_{1}

^{*}

The non perturbative guiding center transformation is extended to the relativistic regime and takes into account electromagnetic fluctuations. The main solutions are obtained in covariant form: the gyrating particle and the guiding particle solutions, both in gyro-kinetic as in MHD orderings. Moreover, the presence of a gravitational field is also considered. The way to introduce the gravitational field is original and based on the Einstein conjecture on the feasibility to extend the general relativity theory to include electromagnetism by geometry, if applied to the extended phase space. In gyro-kinetic theory, some interesting novelties appear in a natural way, such as the exactness of the conservation of a magnetic moment, or the fact that the gyro-phase is treated as the non observable fifth dimension of the
*Kaluza-Klein *model. Electrodynamics becomes non local, without the inconsistency of self-energy. Finally, the gyrocenter transformation is considered in the presence of stochastic e.m. fluctuations for explaining quantum behaviors via Nelson’s approach. The gyrocenter law of motion is the Schr
ödinger equation.

In plasma physics, the gyrokinetic codes are heavily used because they offer the possibility to understand plasma mechanisms from first principles. The collective dynamic is the effect of the self-consistent interaction of single particles with electromagnetic fields. The particle interaction with electromagnetic (e.m.) fields is described by the Lorentz’s force law, whilst the e.m. fields are described by Maxwell’s equations. The difficulty is in the nonlinearity of the problem, because the same e.m. fields that influence the motion of the single particle are sustained by the four-current charge density made by the same particles.

The lagrangian for describing electrodynamics is the sum of the single particle lagrangian, l ( t , x , v ) , times of the distribution function of particles, f ( t , x , v ) , plus the e.m. lagrangian. The action is often expressed as [

S plasma = ∫ d t d x d v f ( t , x , v ) l ( t , x , v ) − ∫ F α β F α β 4 d t d x , (1)

where F α β is the e.m. tensor. This problem is so difficult that some approximations are often considered: the motion of the particles is approximated, e.g. in laboratory plasmas the relativistic effects are neglected and/or the non-uniformity of the magnetic field is ignored. In the present work, we use a non-perturbative approach for describing the particle relativistic motion in a self-consistent e.m. field. Moreover, mainly for astrophysical and cosmic plasmas, the present description is extended to a general relativistic formulation when the presence of a gravitational field is not negligible. It is worth noticing that the solution of an exact Vlasov-Maxwell-Einstein system gives the most complete description of what concerns the classical field theory approach for studying plasmas.

The work is divided in four parts. In the first part, the single particle lagrangian and its Euler-Lagrangian (EL) equations of motion, i.e. the Lorentz’ force law, are studied. In the second part the non-perturbative guiding center description is described, which differs a lot from the standard perturbative approach [

In the third part, it is proposed a method for describing electrodynamics within the general relativity, also for solving the problem of the self-energy. Finally, in the fourth part of this work, electromagnetic fluctuations are considered for obtaining the gyrocenter transformation. The e.m. fluctuations are, firstly, considered as stochastic and the present derivation of the gyrocenter transformation is very different from [

We can begin by noticing that there is an asymmetry in the action (1) between the particle part and the field part. The e.m. action is obtained by integrating the lagrangian density over a definite portion of space-time. This is because Faraday defined a field as an object that depends only on space-time variables, e.g. the magnetic field is B = B ( t , x ) . Differently, in the particle action, the motion of charges is described on the whole phase-space during time evolution. The integration is done over the extended phase-space (the phase space plus time). In principle, for restoring the symmetry between the two lagrangians, matter plus fields, it should be simple to think at an action written as

S plasma = ∫ d t d x d v L plasma , (2)

where L plasma = f ( t , x , v ) l ( t , x , v ) + “ somethingnew ” and the property that

∫ “ somethingnew ” d v = − F α β F α β 4 . (3)

Introducing the phase space lagrangian, which is a lagrangian density over the extended phase-space, L plasma = L plasma ( t , x , v , x ˙ , v ˙ ) , it could be possible to extend to the whole extended phase-space a ( 6 + 1 ) dimensional field theory machinery for studying plasmas.

In the theory of gravitation, a similar symmetry between fields and masses is obtained because the required integration of the lagrangian density is only on a definite portion of space-time, thus the velocity doesn’t effectively matter. The gravitational force doesn’t depend on the velocity of masses even if gravitation determines the motion of masses, thus, also their velocities. In the lagrangian of a neutral massive body, there is not an interaction term like A ⋅ v , depending on the velocity of the body. In general relativity theory, it is possible to think at a consistency between the gravitational field and the motion of masses. Indeed, what is said is that the space-time coincides with the gravitational field in the general relativity theory thanks to the Einstein’s equation. The mass trajectory, the curve in space occupied by the mass during time evolution, is a geodesic on the space-time manifold curved by the presence of masses: the mass can only follow its trajectory consistently with the underlying gravitational field. Is it possible to think at the charge trajectory in a similar fashion? Is it possible to say that the charge trajectory, the curve in phase-space occupied by the charge during time evolution, is the geodesic on the extended phase-space curved by the presence of charges? If yes then it should be possible to obtain an Einstein’s equation also for electromagnetism.

The reason for reviewing some topics of the general relativity theory is that in the third part of the present work we will encounter an Hilbert-Einstein (HE) action, as done in the variational approach for deriving Einstein’s equation in general relativity but, this is done by considering a metric on the whole extended phase-space. It is proposed to substitute the term “something new” in (2) with a HE term when velocities are considered as dynamical variables. In this way, we are able to obtain the self-consistent solution of the problem of electrodynamics concerning plasmas in a general e.m. field. Moreover, having used an HE action we will discover that our solutions are also valid in the presence of a gravitational field. If the correctness of such approach will be confirmed the result is very important because it could be said, from now on, that the gravitational field coincides with the extended phase-space and not only with the space-time. The important difference with the standard approach is that from giving a geometry to the extended phase-space it is possible to obtain gravitation with electromagnetism.

Although an Einstein’s equation on the extended phase-space should be, somehow, analyzed, it will not been studied here. However, it will be analyzed what happens if the (non perturbative) guiding center description of motion is adopted. In such case, a similar mechanism to the one proposed by Kaluza and Klein (KK) a century ago [

In Section II, the basic equations needed for introducing the non perturbative guiding center transformation [

Finally, in Section VI, the particle dynamics are considered with different metric tensors: from a flat space-time geometry ( M 4 ) to a curved extended phase-space (position, velocity and time) geometry. The novelty is that, instead of directly adding to the single particle lagrangian, a term for taking into account the presence of e.m. fields, we prefer to add a HE-like lagrangian. Thus, the metric tensor could be determined through the variation of the HE action in extended phase-space. If the guiding center coordinates are employed, it will be possible to apply the KK mechanism [

The e.m. fluctuations are considered in Section VII and the analysis of solutions, which is the important issue studied in gyrokinetics, is considered here from a stochastic perspective. Thanks to such improvement on the gyrocenter transformation, if non relativistic energies are considered, it will be shown that the gyrocenter motion is fine described by the Schrödinger equation. The possibility of reconciling general relativity with quantum mechanics is resolved by the fact that they describe different quantities, the general relativity describes the guiding center, whereas quantum mechanics describe gyrocenters whose motion, with respect to guiding centers, is also due to electromagnetic fluctuations.

The analysis is firstly done by adopting the Eulerian description of dynamical quantities. However, the final description of motion is done in the guiding center description. Even if the motion is independent on such choice, the privileged reference system here adopted is the guiding center one. In the appendix some details on the derivation of the KK mechanisms are reported following [

A charged particle (charge e and mass m) that moves in a given e.m. field is classically described by the Lorentz’s force law:

d d t γ v v = e m ( E + v × B ) , (4)

for the speed of light set to 1. The relativistic factor is γ v − 1 = 1 − v 2 in the flat Minkowski spacetime. If s is the proper time or the world line coordinate, then γ v − 1 = s ˙ , where the dot is indicating the time derivative. In (4), v = x ˙ is the velocity. To obtain the solutions of (4), we use the newtonian idea of a deterministic world. Following [

d d t γ v v = ∂ t γ v v + v ⋅ ∇ γ v v = ∂ t γ v v + γ v − 1 ∇ γ v 2 v 2 2 − v × ∇ × γ v v . (5)

Introducing the e.m. potentials, Φ and A, in (4) then the Equation (5) becomes

∂ t ( γ v v + e A / m ) + γ v − 1 ∇ γ v 2 v 2 2 + ( e / m ) ∇ Φ = v × [ ( e / m ) B + ∇ × v ] . (6)

From the identities γ v − 1 ∇ γ v 2 v 2 / 2 = γ v − 1 ∇ γ v 2 / 2 = ∇ γ v , it follows:

∂ t ( γ v v + e A / m ) + ∇ ( γ v + e Φ / m ) = v × ∇ × ( γ v v + e A / m ) . (7)

The latter equation can be suggestively read introducing the “canonical” e.m. fields E c = − ( m / e ) ∇ ε − ( m / e ) ∂ t p and B c = ( m / e ) ∇ × p . In fact, E c and B c are said “canonical” because of the potentials, Φ c = ( m / e ) ε and A c = ( m / e ) p , that are the energy and momentum, i.e. the canonical variables of time and position, respectively. Now, the Equation (6) is rewritten as

E c + v × B c = 0 , (8)

which means that in the reference frame that moves with the particle, x ˙ = v ( t , x ) , the particle is seen always at rest. In fact, the resultant of forces vanishes in such co-moving frame. This is the free-fall reference frame for electromagnetism and something similar to the equivalence principle can also be stated here. The difference with the standard approach is that it has been adopted an eulerian description of motion instead of the lagrangian one. The main differences between the two approaches are soon analyzed.

If the charge position at t = 0 is known: x ( t = 0 ) = x 0 , then the flow is represented by the map, Φ t , that determines the charge position at a later time:

x ( t ) = Φ t ( x 0 ) , (9)

being x 0 = Φ t = 0 ( x 0 ) . In continuum mechanics, the former equation is simply named the motion. Concerning the definition of Lagrangian vs Eulerian descriptions, we closely follow the textbook [

a = ∂ t v + v ⋅ ∇ v . (10)

The non relativistic Lorentz’ force law is the same of Equation (4) with the substitution γ v = 1 . It is quite simple to obtain such force from the Euler-Lagrange (EL) equations:

d d t ∇ x ˙ L nr − ∇ L nr = 0, (11)

where the non relatvistic lagrangian, L nr = L nr ( t , x , x ˙ ) , is

L nr ( t , x , x ˙ ) = x ˙ 2 2 + ( e / m ) x ˙ ⋅ A ( t , x ) − ( e / m ) Φ ( t , x ) . (12)

It is remarkable that the EL equations can be obtained from a variational principle, i.e. the Hamilton’s principle. If the action is defined to be

S nr = ∫ t in t out L nr d t . (13)

being t out and t in two different instants of time, then it is possible to associate the EL equations with an extremal of the action. If all the trajectories are considered, from t in and t out , there are some of those trajectories for which the action is at an extremal. Let’s take a trajectory of motion, x = X ( t ) that passes in X in at t in and in X out at t out . Such trajectory is the so-called trajectory of motion because it is solution of X ¨ = ( e / m ) ( E + X ˙ × B ) . Starting from such trajectory it is possible to consider all the other trajectories that are parametrically written at each instant of time, t, as

x = X + ρ ( t , X , α ) (14)

x ˙ = X ˙ + ρ ˙ ( t , X , α ) ,

where α = ( α 1 , α 2 , α 3 ) could vary on a three dimensional domain. It is useful to ask for the following property: if α 2 goes to zero, then also ρ goes to zero and the considered trajectory collapses on the trajectory of motion, x goes to X (and x ˙ goes to X ˙ ). With respect to the standard approach we are considering all the trajectories, not only the one starting from X in at t in to X out at t out . Such difference causes the following consequence. The variation of the action (with respect to the parametric space), δ S nr is always given by

δ S nr = ρ ⋅ ∇ x ˙ L nr | t in t out − ∫ t in t out [ d d t ∇ x ˙ L nr − ∇ L nr ] ⋅ ρ d t , (15)

but now the EL equations doesn’t ensure that δ S nr = 0 because of the term ρ ⋅ ∇ x ˙ L nr which can be different from zero. The common practice is to consider ρ = 0 at t = t in like at t = t out . However, this is not necessary. You can also consider all the trajectories with ρ ⋅ ∇ x ˙ L nr = 0 but ρ ( t in ) ≠ 0 and ρ ( t out ) ≠ 0 , and, again, the result is that the force law corresponds to the vanishing of the first variation of the action. In this case there are many (infinite) trajectories for which the EL equations (i.e. Lorentz’ force law) are satisfied, even if the coordinates X , X ˙ are always describing the unique trajectory that starts from X in at t in to reach X out at t out when α 2 is zero. In such case, both the EL equations and the Hamilton’s principle are satisfied, even if α 2 ≠ 0 . The reason for noting such difference with respect to the standard approach is quite unimportant unless there is something, like an indetermination principle or some non-locality properties, that doesn’t allow to exactly known where the particle is at t in and at t out . We will see in section VI that the present theory is non-local and the latter extended approach to the variational description is useful. Moreover, in section VII, it is shown that α 2 ≠ 0 almost always and the classical trajectory (with α 2 = 0 ) is ruled out by electromagnetic fluctuations.

In (12), it is possible to substitute the potentials, that now are fields, i.e. functions of time and position, with other physically meaningful fields. For an arbitrary velocity field, V ( t , x ) , it is possible to define E ( t , x ) = V 2 / 2 + ( e / m ) Φ and P ( t , x ) = V + ( e / m ) A . Also E = E ( t , x ) and P = P ( t , x ) are fields. The Lagrangian becomes

L nr = x ˙ 2 2 + x ˙ ⋅ ( P − V ) ( t , x ) − ( E − V 2 / 2 ) ( t , x ) = ( x ˙ − V ) 2 2 + P ⋅ x ˙ − E . (16)

The momentum, p ≡ ∇ x ˙ L , is p = x ˙ − V + P .

It is worth noticing that the arbitrariness of V is very important. Behind such arbitrariness there is the relativity principle. In fact, the presence of V can be seen as a particular choice of the reference frame in the space of velocities and, therefore, does not affect the dynamics. It is not important if the observer of an experiment moves with an arbitrary velocity V, the physics described by the experiment remains the same because the lagrangian has the same value, being a scalar. The property of the lagrangian of being a scalar is the relativity principle and it will be very useful in next sections.

Now, it is easy to recognize two different descriptions of the same motion, the Lagrangian description, which is almost adopted, is when V = 0 and the Lorentz’s force law is recovered. Whilst, for x ˙ = V ( t , x ) , the description is said Eulerian.

Concerning the Euler-Lagrange (EL) equations, they are computed:

d d t ( x ˙ − V ) = − ∂ t P − ∇ E + x ˙ × ∇ × P − ( x ˙ − V ) × ∇ × V − ( x ˙ − V ) ⋅ ∇ V . (17)

Introducing the canonical e.m. fields ( e / m ) E c = − ∂ t P − ∇ E and ( e / m ) B c = ∇ × P , the former can be rewritten as

d d t ( x ˙ − V ) = ( e / m ) ( E c + x ˙ × B c ) − ( x ˙ − V ) × ∇ × V − ( x ˙ − V ) ⋅ ∇ V . (18)

It is now evident that a solution of motion is when x ˙ = V and V is solution of Equation (8):

E c + V × B c = 0 , (19)

which seems, only apparently, an algebraic equation.

In dynamical systems or continuum mechanics, given the eulerian velocity field V = V ( t , x ) , i.e. the velocity of the charge when it passes at x at time t, the problem is to find the particle path, integrating the equation x ˙ = V ( t , x ) . Differently, here the eulerian velocity is not given and we have to solve Equation (8) to obtain the velocity field, eventually for trying to integrate the motion (which is not our first interest). We concisely refer to Equation (8) as the velocity law because it can be found for every e.m. fields and for every charge if the eulerian description is adopted. Moreover, with respect to an observer that moves with the Eulerian velocity V ( t , x ) , from Equation (18), the electric field is E c + V × B c which is null so that the charge is kept at rest. With respect to an observer co-moving with the laboratory, the e.m. fields can be measured to be E and B whilst the charge is seen to move following the Lorentz’s force law.

Another interpretation of the same equation, is the following. Suppose to realize, in a laboratory, the electric field, E c , and the magnetic field, B c , and to be able to move the charge in X at t in such a way that its velocity is described by V ( t , X ) . Then, the Lorentz’ force on the particle vanishes, being E c + V × B c = 0 . Without a force on the charge, it is possible to consider the charge velocity preserved as in an inertial reference frame. The problem is that the velocity is not constant and the trajectory is not straight as for a global inertial reference frame. This is exactly what occurs if the reference frame is considered inertial only locally as it happens when an equivalence principle is considered.

It is worth noticing that there is an interesting similarity between such equations of motion and the ideal Ohm’s law encountered in magneto-hydro dynamics (MHD). In MHD, the ideal Ohm’s law is below written: E + V p × B = 0 , being V p the plasma eulerian velocity. Thus, even if the context is different, the solutions are similarly classified (see also [

If B c ≠ 0 , it is possible to rewrite E c + V × B c = 0 as

V = V b b + E c × B c B c 2 , (20)

where b is the unit vector in the direction of the canonical magnetic field, B c = | B c | b , and E c × B c / B c 2 is the E × B -like drift velocity. In plasma physics, it is interesting to study the case corresponding to the gyro-kinetic ordering that neglects the E × B -like drift.

Last but not least, in the Eulerian description the lagrangian in (16) corresponds to the Poicaré-Cartan form, which linearly depends on the velocity:

L P C = P ( t , x ) ⋅ x ˙ − E ( t , x ) . (21)

When relativistic energies are considered it is important to give a covariant description. In this section the spacetime is considered Minkowskian (flat geometry) with signature η α β = diag ( 1, − 1, − 1, − 1 ) . Let’s start from the scalar Lagrangian:

L = − 1 + ( e / m ) ( A ⋅ u − Φ 1 + u 2 ) , (22)

being 1 + u 2 = γ v . We indicate with the prime the derivative with respect to the world line coordinate, s, so that u = x ′ is the relativistic velocity. The lagrangian (22) is the sum of two effects, the free single particle lagrangian is L free = − 1 while the lagrangian expressing the interaction between matter and the e.m. field is L ime = ( e / m ) ( A ⋅ u − Φ 1 + u 2 ) . Adopting the summation convention and for u α u α = 1 with α = 0 , 1 , 2 , 3 , the lagrangian can be re-written in the familiar form

L = − u α ( u α + e A α / m ) , (23)

being A 0 = Φ the electric potential. Explicitly, we have assumed that the contravariant velocity is u α = ( γ v , γ v v ) , while the covariant velocity is obtained from the product u α = η α β u β , that gives u α = ( γ v , − γ v v ) .

From 1 = 1 / 2 + u α u α / 2 , an equivalent lagrangian can be written:

L = − u α u α 2 − e m u α A α − 1 2 . (24)

It is worth to note that such lagrangian is very similar to the non relativistic one, L nr = v 2 / 2 + ( e / m ) ( v ⋅ A − Φ ) ; if u → v then the difference is only due to the energy at rest, which is absent in L nr .

Now, for an arbitrary four co-variant velocity field, U α = U α ( x β ) it is possible to define a co-vector field, P α = P α ( x β ) = U α + ( e / m ) A α . The Lagrangian becomes

L = − u α u α 2 − u α ( P α − U α ) − 1 2 . (25)

The four co-momentum are

p α = − ∂ L ∂ u α = u α + P α − U α . (26)

The EL equations are simply

d d s p α = u β ∂ α ( P β − U β ) , (27)

that, finally, can be written as:

d d s ( u α − U α ) = u β ( ∂ α P β − ∂ β P α ) − u β ∂ α U β . (28)

As before, if U α = 0 the equations of motion give the covariant Lorentz’s force law, and a Lagrangian description is preferable. However, if u α = U α ( x β ) , then the description is Eulerian. In the Eulerian description, the Eulerian four velocity satisfy the Equation (8) because u α u α = 1 and u β ∂ α u β = 0 . The velocity law can be written in co-variant form as

u β ω α β = 0 , (29)

being ω α β = ∂ α P β − ∂ β P α , known as the Lagrange tensor.

The canonical Maxwell tensor, F c α β is proportional to the Lagrange tensor, ω α β :

( e / m ) F c α β ≡ ω α β = ∂ α P β − ∂ β P α . (30)

Thus, Equation (8) is found when α = 1 , 2 , 3 ; whilst, if α = 0 then

γ v v ⋅ ( − ∇ E − ∂ t P ) = 0, (31)

which means that E c is transversal to v, so that it doesn’t contribute to the energy variation (for this reason, in [

Even if we have already obtained the covariant equations, it is instructive to derive the same Equation (29) directly from the most simple lagrangian: L = − u α p α ( x β ) , which is the same of (23) but now the covariant momentum, p α = p α ( x β ) , is only function of the spacetime coordinates and it doesn’t depend on the (relativistic) velocity (its one-form is the Poincaré-Cartan form). For such lagrangian, the four momentum is

p α ( x β ) ≡ − ∂ ∂ u α L (32)

and the EL equations are:

u β ∂ β p α = u β ∂ α p β , (33)

being p ′ α = u β ∂ β p α . The former is exactly the Equation (29).

There are some simple solutions of the Equation (29). The trivial solution, ω α β = 0 , results to be very important. Another simple solution is ω α β = ϵ α β γ δ k γ u δ , where ϵ α β γ δ is the Levi-Civita symbol ( ϵ 0123 = 1 ) and k γ is the wave number four-vector. Also this solution is trivial because the Levi-Civita symbol is totally anti-symmetric, so that u β ϵ α β γ δ k γ u δ = 0 due to the symmetry β ↔ δ .

From Equation (20) it is possible to classify the solutions of the velocity law depending on 1) B c = 0 and E c = 0 , 2) B c ≠ 0 and E c = 0 and 3) B c ≠ 0 and E c ≠ 0 . They are called, gyrating particle solution, guiding particle solution in gyrokinetics ordering and guiding particle solution in MHD ordering, respectively.

Let’s start with the analysis of the following solution: ω α β = ϵ α β γ δ k γ u δ and consider the case k 0 = 1 / λ and k = 0 . Now, ω α β = u δ ϵ δ α β 0 / λ . Thus, only the spatial components survive:

ω i j = u k λ ϵ i j k with i , j , k = 1 , 2 , 3. (34)

Multiplying for ϵ i j l both sides of the latter equation, and using the equivalence ϵ i j k ϵ i j l = 2 δ k l , then

u l λ = ϵ i j l 2 ω i j = ϵ i j l ∂ i p j , (35)

which is the l component of the fundamental equation:

u λ = e m B + ∇ × u , (36)

as in the non-relativistic case [

The latter equation is said fundamental because its solution gives the answer for many problems encountered in plasma physics and/or electrodynamics. At first, if λ → ∞ then B = − ( m / e ) ∇ × u and the velocity becomes strictly related to the vector potential: the problem is to find a vector potential from a given magnetic field. This kind of solution will be called the gyrating particle solution. Secondly, if ( e / m ) → 0 then u = λ ∇ × u , which is recognized as the force free equation [

^{1}In the present case S = W − ε t , where W is the Hamilton’s characteristic function and ∇ S = ∇ W .

Nevertheless, written in the latter form, something unusual appears. In fact, the Hamilton-Jacobi solutions, that are classical solutions, are obtained setting p = ∇ S , where S is the principal Hamilton function^{1}. In our case, p is not a gradient of a function, otherwise its curl should vanish. We have already defined the canonical magnetic field exactly as the curl of ( m / e ) p . This means that classical solutions have B c = 0 and so, we are inspecting non classical solutions with B c ≠ 0 .

Together with (36), there is also the condition ω 0 i = 0 , which means:

∂ t p + ∇ ε = 0 , (37)

as it should in the gyrokinetic-like ordering ( E c = 0 ). Such equation, already studied in [^{th} order approximation is

U ( 0 ) = e m λ B . (38)

The leading order approximation is

U ( 1 ) = λ e m B + λ ∇ × U ( 0 ) . (39)

If λ = ( m / e ) u ∥ / | B | , then the former is the familiar guiding center (relativistic) velocity (for null magnetic moment) at leading order:

U ( 1 ) = u ∥ b ( 0 ) + u ∥ ( e / m ) | B | ∇ × u ∥ b ( 0 ) , (40)

with B = | B | b ( 0 ) . In [

B = ∇ ψ p × ∇ ϕ + F ∇ ϕ , (41)

where ϕ is the toroidal angle, ψ p is the poloidal magnetic flux surface and F/R is the toroidal component of the magnetic field ( ∇ ϕ = e ϕ / R with e ϕ , the unit vector in the toroidal direction, and R the radial distance from the axis). The guiding particle velocity solution of (36) in an axisymmetric magnetic field like (41) is [

U = λ e m ∇ P ϕ × ∇ ϕ + e m ( P ϕ − ψ p ) ∇ ϕ (42)

with the guiding particle toroidal momentum, P ϕ (in magnetic flux unit), satisfying the following equation:

λ R 2 ∇ ⋅ λ ∇ P ϕ R 2 + P ϕ = 0, (43)

if λ = − ψ p / F . The latter equation, that can be written as an eigenvalue equation for the Shafranov operator, was already obtained but wrongly written in [

Previously, we have analyzed the following solution of the velocity law: ω α β = ϵ α β γ δ k γ u δ , with k γ the time-like four-vector: k 0 = 1 / λ and k = 0 . We have noticed that from this choice it follows that E c = 0 , which is said the gyro-kinetic-like ordering. Now we want to consider the case where k γ is the space-like four vector ( 0, k ) . In such case, ω α β = ϵ α β i δ k i u δ = ϵ α β i 0 k i u 0 + ϵ α β i j k i u j . The component of ω α β are

ω 0 k = ϵ 0 k i j k i u j = ( k × u ) k (44)

and

ω k j = ϵ k j i 0 k i u 0 . (45)

That can be written in vectorial form as

E c = ( m / e ) γ v k × v (46)

and

B c = ( m / e ) γ v k , (47)

being ω α β = ( e / m ) F c α β . In such case it is the wave number, and not v, that is parallel to B c . The solution for v is the same of (20) but contrary to before the particles don’t follow trajectories close to the magnetic field lines because of the presence of the electric field E c . This is what happens in the MHD-like ordering. Thus, we can easily distinguish the MHD-like from the gyrokinetic ordering giving to k σ the character of a space-like or time-like four-vector, respectively. The same conclusion can also be done if the ideal Ohm’s law is considered instead of the velocity law of Equation (8).

The trivial solution of (29) is ω α β = 0 . In such case the canonical fields are null: F c α β = 0 , or E c = B c = 0 .

If B c = 0 , then ( e / m ) B + ∇ × u = 0 . Now, it is possible to choose a very particular vector potential: A = − ( m / e ) u + ∇ g , being g a gauge function. Moreover, the function g is also seen to be proportional to the principal Hamilton’s function, S, which is an action. Indeed, the canonical momentum is p = u + ( e / m ) A = ( e / m ) ∇ g . If g = ( m / e ) S , then p = ∇ S and we have just set the initial condition for finding the classical solution in the Hamilton-Jacobi method. This is also consistent with E c = 0 , that means that ∇ u 0 + ( e / m ) ∇ Φ + ( e / m ) ∂ t ∇ g = 0 . If ε = u 0 + ( e / m ) Φ = − ( e / m ) ∂ t g , then we found the other Hamilton-Jacobi equation: ε + ∂ t S = 0 , being S = ( e / m ) g .

The gyrating particle solution is the most important solution. The reason will only be clear in Section VII, but it is possible to notice some interesting properties also here if the gauge function is settled to g = ( m / e ) 2 μ γ (such choice will soon be defined as the guiding center gauge function). The four-vector co-momentum is p α = − ( m / e ) μ ∂ α γ . Explicitly, p = ( m / e ) μ ∇ γ and ε = − ( m / e ) μ ∂ t γ .

Such solution allows to compute the Lagrangian, whose value is: L = v ⋅ p − ε = ( m / e ) μ ( ∂ t γ + v ⋅ ∇ γ ) = ( m / e ) μ γ ˙ . If γ is the gyro-phase, the conjugate coordinate, μ , is the magnetic moment. Thus, the gyrophase comes to be proportional to the action. Such remark was already considered by Varma [

ε = [ p − ( e / m ) A ] 2 2 + e m Φ . (48)

it can be re-written in an interesting way once the phase function, ψ zbw = e − i γ , is considered. Here, zbw stands for Zitterbewegung [

∇ ψ zbw = − i ψ zbw ∇ γ and ∂ t ψ zbw = − i ψ zbw ∂ t γ . (49)

Thus, the momentum and the energy can be written as

p = i ( m / e ) μ ψ zbw ⋆ ∇ ψ zbw , (50)

ε = − i ( m / e ) μ ψ zbw ⋆ ∂ t ψ zbw , (51)

where ψ zbw ⋆ indicates the complex conjugate of ψ zbw , which, in this case, it is also the inverse: ψ zbw ⋆ = ψ zbw − 1 . The energy is computed:

− i ( m / e ) μ ψ zbw ⋆ ∂ t ψ zbw = e m Φ + 1 2 [ i ( m / e ) μ ψ zbw ⋆ ∇ ψ zbw − ( e / m ) A ] ⋅ [ − i ( m / e ) μ ψ zbw ∇ ψ zbw ⋆ − ( e / m ) A ] ,

being p and ε real quantities. The former expression is written as

− i ( m / e ) μ ψ zbw ⋆ ∂ t ψ zbw = e m Φ + ψ zbw ⋆ [ i ( m / e ) μ ∇ − ( e / m ) A ] 2 2 ψ zbw + i 2 ∇ ⋅ [ i ( m / e ) μ ψ zbw ⋆ ∇ ψ zbw − ( e / m ) A ] .

The divergency term is ∇ ⋅ v and it is null for an incompressible charge, neither created nor destroyed. A Schrödinger-like equation is obtained:

− i ( m / e ) μ ∂ t ψ zbw = [ i ( m / e ) μ ∇ − ( e / m ) A ] 2 2 ψ zbw + e m Φ ψ zbw . (52)

The operator, of the former partial differential equation, is exactly the same of the Schrödinger equation if e < 0 , as for an electron, and μ = | e | ℏ / m 2 . From totally classical assumptions, the expression of the energy for a charged particle together with the constrain that ∇ ⋅ v = 0 , give rise to a wave equation. Thus, for a gyrating particle solution it is possible to describe a classical solution of motion through a Schrödinger equation applied to a phase function like ψ zbw . It is interesting that there is a set of solutions where both the Schrödinger-like equation and the Lorentz’s force law are verified. What is important is that determinism is preserved by the fact that | ψ zbw | = 1 , which means, in the Born interpretation of | ψ zbw | 2 , that the probability of finding the particle in the state represented by ψ zbw is almost certain (only if you know the initial gyrophase).

For the gyrating particle solutions, it is possible to take the following representation for the magnetic field: B = ∇ Ψ × ∇ γ , which is commonly called Clebsh representation. Ψ and γ are said Clebsh potentials. Topologically, it is possible to choose γ ∈ S 1 , in such a way that, in this case, it is considered the gyro-phase. The variable Ψ is the magnetic flux linked to the closed loop traced by γ . ∇ Ψ is orthogonal to ∇ γ , in such a way that B doesn’t depend on γ . The particle, that travels along the closed loop of curvilinear coordinate γ , always feels the same orthogonal magnetic force. This happens for the particular representation of the magnetic field, not because the magnetic field is straight and uniform. For this reason, such representation is also known as the straight field line representation. The motion of the gyrating particle is expressed by:

x = X + ρ (γ)

u = U + ν ( γ ) = ν ( γ ) ,

where we have set U = 0 , so that the guiding center, X, is fixed. The gyrating loop motion has been described in [

ν = ρ × Ω , (53)

where Ω is the relativistic angular frequency vector, that depends on the position of the particle. It is possible to choose a local tern of orthogonal unit vectors: e γ ⋅ e ρ × b = 1 , where ρ = | ρ | e ρ , Ω ⋅ b = γ ′ and ν = | ρ | γ ′ e γ .

It is worth noticing that | ρ | becomes a conserved quantity if (53) is allowed. In fact, the world line derivative of ρ 2 / 2 is ρ ⋅ ρ ′ = ρ ⋅ ρ × Ω = 0 . Thus, | ρ | doesn’t depend on γ . However, | ρ | depends on the magnetic flux linked to the closed orbit. In other words, distances are now measured in terms of Ψ . Moreover, also the time of one revolution depends on Ψ , so that it can be considered a good time-like coordinate.

From (53), the closed trajectory lives on the surface of a sphere, S 2 , of radius | ρ | . However, if other coordinates are used then the same particle is seen to move on a helicoidal trajectory. The circle S 1 is both the representation of the particle orbit, but also the description of the gyrating motion in the guiding center coordinates. What is important is that there is no difference from the point of sight of the particle. The particle moves in a circle, ignoring the rest of the world because it can only feel the effect of the Lorentz’ force with the same magnetic field intensity. If the charge is described in the guiding center reference frame, then the magnetic field is always orthogonal to its direction of motion. In a certain sense, it is similar to a massive body in a gravitational field: the massive body moves straight along the geodesic but the spacetime is curved due to the presence of a gravitational field and the body is seen from an observer, e.g. to fall versus another massive body. On the same footing, a charged particle moves circularly but the spacetime is measured in units of magnetic field and if such magnetic field is non uniform then the charge is seen from an observer with a relative relativistic velocity − U ≠ 0 , e.g. to follow a helicoidal trajectory. In the forthcoming sections, the guiding center description of motion will be described, when both U and ρ are not vanishing, and it will be shown how the electromagnetism can be described within the formalism of general relativity.

Here, another interesting and important description of motion is considered, with respect to the Eulerian and the Lagrangian descriptions: the guiding center description of motion which is neither Lagrangian nor Eulerian. Such possibility arises if the velocity of the charge is written as x ˙ = V + σ . Now, the motion is not Eulerian, because V ≠ x ˙ , and it doesn’t express the velocity of the charge at a given time and position. V expresses the velocity field that is used as a system of reference for velocities measured by σ = x ˙ − V . Such description is not Lagrangian, because V ≠ 0 , now. However, if the vector field σ is defined on the same domain of V, then re-naming V ˜ = V + σ , the description can be done in the Lagrangian or Eulerian way, as previously done. Instead, for the guiding center description we do something different, now σ depends on a new variable or parameter, γ ∈ S 1 , which it can be identified with the gyro-phase. In practice, γ must live in a different domain from the one where the e.m. fields are defined and, thanks to Faraday, the e.m. field only varies on space-time. Such new variable is always part of the whole phase-space. The non perturbative guiding center transformation is the transformation from ( t , x , v ) to ( t , X , γ , μ , ε ) , where μ is the magnetic moment, that will be defined later on, whilst ε is the energy of the charge. The transformation is implicitly written as

x = X + ρ ( t , X , γ ; μ , ε ) (54)

v = V ( t , X ; μ , ε ) + σ ( t , X , γ ; μ , ε ) .

The latter relations are considered at each time, t, and express the trajectory of the charge through the guiding center coordinates ( t , X , γ , μ , ε ) . Comparing such relations with the parametrized trajectories in (14), it is straightforward to identify α with α = ( γ , μ , ε ) . Specifically α 1 = γ , α 2 = μ and α 3 = ε . In (54), ρ is the gyro-radius and X is the guiding center position. The guiding center velocity is X ˙ = V , if V is computed at X.

The contra-variant guiding center coordinates are Z A = ( t , X , γ , μ , ε ) , with the index A from 0 to 6. The coordinates Z A are contra-variant because they transform in the following way: if Z A = Z A ( z B ) then

d Z A = ∂ Z A ∂ z B d z B . (55)

In the guiding center description of motion the single particle lagrangian doesn’t depend on γ , therefore, a reduction of the complexity of the problem is achieved: γ is cyclic and the conjugate variable, that is the magnetic moment, μ , becomes an invariant of motion. The lagrangian in (12) is rewritten by separating the guiding center part:

L nr ( t , X + ρ , V + σ ) = ( V + σ ) 2 2 + ( e / m ) ( V + σ ) ⋅ ( A + δ ρ A ) − ( e / m ) ( Φ + δ ρ Φ ) ,

where A ( t , x ) = A ( t , X ) + δ ρ A and Φ ( t , x ) = Φ ( t , X ) + δ ρ Φ . Here, V is always solution of Equation (19) for ensuring that if μ → 0 then V describes the velocity of a particle. The lagrangian is written in such a way that it is divided in what surely doesn’t depend on γ , firsts three terms below, from what it should:

L nr = V 2 2 + ( e / m ) V ⋅ A − ( e / m ) Φ + P ⋅ σ + ( e / m ) ( V ⋅ δ ρ A − δ ρ Φ ) + σ 2 2 + ( e / m ) ( σ ⋅ δ ρ A ) .

It is advantageous denoting L nr0 = V 2 / 2 + ( e / m ) V ⋅ A − ( e / m ) Φ , as the leading order lagrangian, with L nr1 = P ⋅ σ + ( e / m ) [ ρ ⋅ ( ∇ A ) ⋅ V − ρ ⋅ ∇ Φ ] , as the first order lagrangian, and the rest with L nr2 = L nr − L nr0 − L nr1 . The reason is that the equation of motions are obtained only if the first order lagrangian vanishes. This it can be easily seen if ρ and σ are considered small. In such case L nr2 can be ignored and L nr1 = ρ ⋅ ( e / m ) [ ( ∇ A ) ⋅ V − ∇ Φ − P ˙ ] + d ( ρ ⋅ P ) / d t . The equation of motion are obtained when it is required that L nr1 − ( d / d t ) ( ρ ⋅ P ) = 0 , if the identity ( ∇ A ) ⋅ V = V × ∇ × A + V ⋅ ∇ A is used. This is equivalent to ask for the action to be at an extremal since, neglecting the small variation, ρ , of the trajectory, L nr = L nr0 .

The single particle lagrangian is gauge independent and, for a gauge function g, then the transformation A → A − ∇ g and Φ → Φ + ∂ t g leaves the trajectories of motion unaltered. Indeed, together with the gauge transformation of e.m. potentials the lagrangian is shifted, L nr → L nr − ( e / m ) g ˙ , and the addition of a total time derivative doesn’t affect the EL equations of motion. However, it is common practice to use a gauge function that depends on space and time only. Here, we use a gauge function that depends on the guiding center coordinates. It is worth noticing that quantum mechanics forbids the dependency of e.m. potentials from the velocities by limiting the domain of the gauge function only to the whole space-time. Even though the redefinitions of e.m. potentials doesn’t affect the e.m. field (E and B), it is now possible to cancel or add some terms in the lagrangian that depend on all the variables of the whole phase space, like γ . The dependency of γ in the single particle lagrangian can be manipulated through an efficient choice of the gauge [

( e / m ) g ˙ = − P ⋅ σ − ( e / m ) ( V ⋅ δ ρ A − δ ρ Φ ) − σ 2 2 − ( e / m ) ( σ ⋅ δ ρ A ) . (56)

Moreover, if ∂ γ g ˙ = 0 then the lagrangian

L ˜ nr = V 2 2 + ( e / m ) V ⋅ A − ( e / m ) Φ − ( e / m ) g ˙ (57)

doesn’t anymore depend on γ .

However, the former relation denotes something really important, the equivalence of

p ⋅ v − ε = P ⋅ V − E − ( e / m ) g ˙ , (58)

being ε = v 2 / 2 + ( e / m ) Φ ( t , x ) and E = V 2 / 2 + ( e / m ) Φ ( t , X ) . From the former relation it is clear the reason for indicating ( e / m ) g as the (Lie) generating function for the guiding center transformation. In the non perturbative guiding center transformation it is chosen to set ε = E + ( e / m ) g ˙ and the product p ⋅ v is conserved: P ⋅ V = p ⋅ v . From the linear dependency of the energy on g ˙ , it seems that the energy of the particle should depends also on the chosen gauge. This is what it commonly happens because the energy is linearly dependent on the electric potential which itself is gauge dependent. However, it could be nice if the energy becomes independent from the gauge function, g. This means that ∂ g g ˙ = 0 . In fact, we have just seen that for asking γ to be cyclic in the lagrangian, then ∂ γ g ˙ = 0 . Thus, a simple identification occurs: g ∝ γ . Let’s introduce the magnetic moment as the constant useful for identifying the gauge function with the gyro-phase:

g = ( m / e ) 2 μ γ , (59)

then

ε = E + ( m / e ) μ γ ˙ . (60)

At the same time, it is found from the transformation in (54) that

ε = E + σ 2 2 + σ ⋅ V + ( e / m ) δ ρ Φ . (61)

Comparing the latter relations, the definition of the cyclotron (angular) frequency, ω c = γ ˙ , is:

ω c = σ 2 / 2 + σ ⋅ V + ( e / m ) δ ρ Φ ( m / e ) μ , (62)

and it doesn’t depend on γ , because γ has been imposed to be cyclic for construction. It is quite easy to demonstrate that the magnetic moment is the constant of motion associated to the cyclic variable γ . In this way we have constructed a constant magnetic moment. Its constancy has not been explicitly derived but required for consistency from the following property: the gauge independency of electrodynamics.

The gauge transformation is

A → A − ( m / e ) μ ∇ γ and Φ → Φ + ( m / e ) μ ∂ t γ (63)

also for the relativistic case.

The relativistic transformation is implicitly written as

x = X + ρ ( t , X , γ ; μ , ε ) (64)

u = U ( t , X ; μ , ε ) + ν ( t , X , γ ; μ , ε ) ,

being u = x ′ , U = X ′ and ν = ρ ′ . The relativistic lagrangian is:

L = − u α u α 2 − e m u α A α ( t , x ) − 1 2 . (65)

Once u 0 = γ v has been considered, it is convenient to introduce U 0 and ν 0 . The guiding center velocity is not the velocity of a charge, so that U α U α ≠ 1 if ν α ≠ 0 . Indeed, it is possible to ask for ν α ν α = 0 . In such case ν α is a light-like four-vector, as for a photon. Such correspondence is stressed writing U α = w α − η α , with η α η α = 0 , as for ν , and w α w α = 1 , as for a charge. Now, it is possible to re-write the guiding center four-velocity transformation, u α = U α + ν α , in the following way:

u α + η α = w α + ν α . (66)

The advantage is that it is possible to obtain the correspondence with the conservation of energy and momentum in the Compton-like scattering ( e − + γ → e − + γ ). It is worth noticing that the role of the guiding center is equivalent to the virtual particle in particle physics, now. From such correspondence it is possible to easily obtain the relation between ν 0 and η 0 like for the frequencies involved in the Compton scattering: if η ⋅ ν = η 0 ν 0 cos θ and w α = ( 1 , 0 , 0 , 0 ) , then

η 0 = ν 0 1 + ν 0 ( 1 − cos θ ) , (67)

and

U 0 = w 0 − η 0 = 1 − ν 0 cos θ 1 + ν 0 ( 1 − cos θ ) , (68)

being ν 0 = ± | ν | and, from U 0 + ν 0 = γ v ,

cos θ = 1 − γ v − 1 ν 0 ( γ v − ν 0 ) . (69)

The gauge function, g, should be chosen in such a way that the equivalence in (58) is replaced by

L = − p α u α = − P α U α − ( e / m ) g ′ . (70)

Thus, after a gauge transformation, the product u α p α is not an invariant anymore. Here, it is possible to anticipate what it will be crucial in the KK model: if you assign the values z 0 = t , z = X , z 4 = γ and w 0 = P 0 = U 0 + ( e / m ) Φ , w = P = U + ( e / m ) A and w 4 = ( m / e ) μ , then

L = − w a z ′ a , for a = 0 , 1 , 2 , 3 , 4. (71)

which is a scalar product in a space-time of five dimensions. Moreover, if you require that w 5 = w 6 = 0 and z 5 = μ , z 6 = ε , then you can also write

L = − w A z ′ A , for A = 0 , 1 , 2 , 3 , 4 , 6. (72)

The latter is what is called the phase-space lagrangian from which it is possible to find the Hamilton’s equations. It is better to denote with a tilde the guiding center phase-space lagrangian: L = L ˜ ( z A , z ′ B ) , for A , B = 0 , 1 , 2 , 3 , 4 , 6 . As said in [

Now, the lagrangian is invariant at a glance with respect to general non-canonical phase-space coordinates transformations, that include also the gauge transformations.

Following the work of Cary and Littlejohn [

δ W = δ ∫ s in s out d s p ( x ) ⋅ d x d s = 0. (73)

with p ( x ) = u ( x ) + ( e / m ) A ( x ) and p ( x ) ⋅ δ x = 0 at the end points. The EL equations are

d x d s × ∇ × p ( x ) = 0 , (74)

which means that the velocity u is parallel to ∇ × p ( x ) or

u = λ ∇ × p ( x ) , (75)

re-obtaining the fundamental Equation (36).

The lagrangian p ( x ) ⋅ u is missing something. Now, we explicitly consider the time and the variation of the time dependent action:

δ S = δ ∫ s in s out d s [ p ( t , x ) ⋅ d x d s − ε ( t , x ) d t d s ] = 0. (76)

The variation can be computed as

δ S = ∫ s in s out d s δ x ⋅ ∇ [ p ( t , x ) ⋅ d x d s − ε ( t , x ) d t d s ] + ∫ s in s out d s δ t ∂ t [ p ( t , x ) ⋅ d x d s − ε ( t , x ) d t d s ] + ∫ s in s out d s [ δ d x d s ⋅ p ( t , x ) − δ d t d s ε ( t , x ) ] .

In the present notation, δ x = ρ and δ t = ρ 0 . In covariant notation, such variation is

δ S = ∫ s in s out d s ρ α u β ( ∂ β p α − ∂ α p β ) + ( ρ α p α ) | s in s out . (77)

The extremals of the action, δ S = 0 , for all the trajectories with ρ α p α = 0 (at least at s in and s out ), are found if

u β ( ∂ β p α − ∂ α p β ) = 0 , (78)

which is (29).

Up to now, we have referred to the guiding particle as the particle satisfying (29), or (78), with null magnetic moment (and minimally coupled with the magnetic field). The same Equations (29), or (78), is considered as the equation describing the guiding center velocity if the particle has a non vanishing magnetic moment. In such case we use capital letters e.g. for describing the position X, the velocity V = X ˙ and the four-momentum P α = ( E , − P ) , of the guiding center.

We can add or subtract to the lagrangian a total world line derivative without changing the equation of motion and preserving the scalar value of the Lagrangian. We subtract to L = P ⋅ U − E U 0 the total derivative of the following gauge function:

g = ( m / e ) 2 μ γ , (79)

being μ the constant magnetic moment and γ the gyro-phase.

The new lagrangian is L ˜ = P ⋅ U − E U 0 − ( e / m ) g ′ = P ⋅ U − E U 0 − ( m / e ) μ γ ′ . With respect to the lagrangian L = P ⋅ U − E U 0 , L ˜ is known as (minus) the Routhian, which is defined through the Legendre transformation of L with respect to the cyclic coordinate γ :

− L ˜ ≡ ( m / e ) μ γ ′ − L . (80)

The properties of L ˜ are to combine the EL and the Hamilton’s equations together for describing the motion:

d d s ∇ U L ˜ − ∇ X L ˜ = 0. (81)

and

( e / m ) ∂ μ L ˜ = γ ′ , ∂ γ L ˜ = − ( m / e ) μ ′ , (82)

respectively. The use of the Legendre transformation for the cyclic variable has been used for describing the motion with the coordinates γ , μ instead of γ , γ ′ . Being γ cyclic, μ ′ = 0 in (82).

The present and the next paragraphs are quite technical, but it is important to describe what concerns the dimensional reduction of a system. Historically, the dimensional reduction was a technique used to attack a complicated problem by progressively reducing it in order to reach a resolvable system. In gyro-kinetic the dynamic of the particle is separated from the fast gyro-motion reducing the analysis to the dynamic of the guiding center (if fluctuations are turned off). In the KK mechanism [^{th} dimension unobservable. Thus, the Routhian reduction scheme [

The idea, originally proposed by [

L ˜ d s ˜ = P d X − ( m / e ) μ d γ − E d t . (83)

For such system the motion is described by the variables z a = ( t , X , γ ) , with index a from 0 to 4, so that the world line coordinate, s ˜ , is function of z a : s ˜ = s ˜ ( z a ) . Moreover, the conjugate momenta, w a , are easily introduced consistently with the lagrangian in (83): w a = ( E , − P , ( m / e ) μ ) . Now,

L ˜ = − w a z ′ a , for a = 0 , 1 , 2 , 3 , 4. (84)

However, following the analysis done in [

L ^ d s ^ = − w A d z A , for A = 0 , 1 , 2 , 3 , 4 , 5 , 6. (85)

The scalar character of the lagrangians, (84) like (85), is always preserved and it is possible to change coordinates from z A → Z A and w A → W A leaving unaltered the Poincaré-Cartan form: − w A ( z B ) d z A = − W A ( Z B ) d Z A . This means that the principle of relativity is generalized to the extended phase space: a change of coordinates of the extended phase space preserves the physics.

The EL equation for (85) are

ω A B d z B d s ^ = 0 , (86)

with

ω A B = ∂ A w B − ∂ B w A . (87)

Multiplying Equation (86) for d s ^ / d t , it is found what it can be called the velocity law (compare (29) with (86)) in 7 dimensions (or 5 dimensions if the motion is described through ε and μ , if ε ′ = μ ′ = 0 ). It is worth noticing that a canonical Maxwell tensor in 7 dimensions is proportional to ω A B . The generalized angular frequency tensor, ω A B , is known as the Lagrange tensor. The Lagrange tensor is expressed by the Lagrange’s brackets:

[ z A , z B ] ≡ ∂ A w C ∂ B z C − ∂ B w C ∂ A z C = ∂ A w C δ B C − ∂ B w C δ A C = ω A B (88)

where [ z A , z B ] are the Lagrange brackets.

It is convenient to normalize z ˙ 0 = 1 in (86), which means choosing z 0 = t . Three properties of motion must be reminded: 1) det ( ω A B ) = 0 , from (86), 2) the gauge invariance of motion if w A → w A + ∂ A g , from (87), and 3) in (86) the case A = 0 is redundant due to the antisymmetry of ω A B .

Equation (86) can be arranged to

ω A 0 + ∑ B = 1 6 ω A B z ˙ B = 0 , (89)

with

ω A 0 = ∂ A w 0 − ∂ t w A = ∂ A E − ∂ t w A . (90)

For obtaining the Hamilton’s equations of motion it occurs introducing the antisymmetric Poisson tensor, J A B , with the property that

∑ C = 1 6 J A C ω C B = − δ B A , if A ≠ 0 and B ≠ 0 (91)

Now, the expression in (89), with Equation (90), becomes

z ˙ A = ∑ C = 1 6 J A C ( ∂ C E − ∂ t w C ) if A ≠ 0. (92)

The latter are the Hamilton’s equations of motion for non-canonical coordinates and it can be reduced to

z ˙ A = { z A , E } + ∂ t z A . (93)

if canonical coordinates are employed, being { z A , z B } the Poisson brackets.

Within the guiding center description, when guiding center coordinates, z A = ( t , X , γ , μ , ε ) and w A = ( E , − P , ( m / e ) μ ,0,0 ) , are used, the Lagrange tensor is:

| ( e / m ) F α β c 0 − ∂ μ P α − ∂ ε P α 0 0 − m / e 0 ∂ μ P β m / e 0 0 ∂ ε P β 0 0 0 | (94)

The equations of motion, from (86), are

| ( e / m ) F c α β 0 − ∂ μ P α − ∂ ε P α 0 0 − m / e 0 ∂ μ P β m / e 0 0 ∂ ε P β 0 0 0 | | V β γ ˙ μ ˙ ε ˙ | = 0 (95)

Explicitly, the system of equations of motion is:

( e / m ) F c α β V β − μ ˙ ∂ μ P α − ε ˙ ∂ ε P α = 0 (96)

− ( m / e ) μ ˙ = 0 (97)

V β ∂ μ P β + ( m / e ) γ ˙ = 0 (98)

V β ∂ ε P β = 0 , (99)

where the Equation (99) is redundant for the antisymmetry of F c α β in Equation (96). If also ε ˙ = 0 then

E c + V × B c = 0 (100)

μ ˙ = 0 (101)

V ⋅ ∂ μ P = ( m / e ) γ ˙ ( 1 − V 0 ) (102)

V ⋅ ∂ ε P = V 0 , (103)

If V 0 = 1 then V ⋅ ∂ μ P = 0 and V ⋅ ∂ ε P = 1 .

It is worth noticing that all the lagrange brackets involving γ and μ are null, [ μ , γ ] apart, which is equal to m / e . This is the reason that allows reducing the particle motion ignoring the gyro-phase coordinate, γ , which is said cyclic.

In the perturbative approach of the guiding center transformation a completely different procedure is often used. Moreover, the perturbative approximation is treated with the highly technical Lie-transformation method without solving some ambiguities. For such reason it is often hard to overcome the leading order approximation. However, in the present work, we do not consider a comparison between the two distinct methods, the perturbative and the non-perturbative one. Here, we need only the first order approximation for explaining why μ is the magnetic moment and γ is the gyrophase.

The guiding center lagrangian used in the perturbative approach is the leading order approximation of L g c , which is the lagrangian in (21) associated to the Poincaré-Cartan one-form:

L g c = L nr + ( e / m ) g ˙ = P ⋅ X ˙ − E . (104)

Explicitly,

L g c = p ⋅ x ˙ − ε + ( m / e ) μ γ ˙ , (105)

being g = ( m / e ) 2 μ γ , the guiding center gauge function in (79). Setting ε = E + ( m / e ) μ γ ˙ , as in (60), then

L g c = P ⋅ X ˙ − ε + ( m / e ) μ γ ˙ . (106)

The orderings, which are commonly employed, are the ones that allow to consider the particle close to the magnetic field line, in such way that field lines deviate only linearly from being straight and uniform (this is quite a rough approximation but almost always used). Within such orderings, the charges are gyrating circularly around the guiding center. Once the tern of unit vectors, e 1 ⋅ e 2 × b ( 0 ) = 1 , are defined with b ( 0 ) ⋅ B = | B | parallel to the magnetic field, the guiding center is considered mostly moving in the parallel direction of the magnetic field in such a way that P is substituted with P ≈ v ∥ b ( 0 ) + ( e / m ) A ( t , X ) . The gyro radius can be written as

ρ ≈ a ( 0 ) = ρ L ( e 1 cos γ − e 2 sin γ ) , (107)

with the constant Larmor radius, ρ L . It is worth noticing that γ is the angle in the cylindrical representation of the velocity space. If γ ˙ = ( e / m ) | B | , which is the important cyclotron frequency, then

v ⊥ ≈ a ˙ ( 0 ) = − ρ L γ ˙ ( e 1 sin γ + e 2 cos γ ) = ( e / m ) a ( 0 ) × B . (108)

Commonly the electric potential is neglected and the energy of the charge is the only kinetic energy:

ε = v 2 / 2 . (109)

Moreover, the problem is often considered static: A = A ( X ) with ∂ t A = 0 . The single particle lagrangian,

L = [ v ∥ b ( 0 ) + v ⊥ + ( e / m ) A ] ⋅ x ˙ − ε , (110)

is approximated by

L ≈ ( v ∥ b ( 0 ) + a ˙ ( 0 ) ) ⋅ ( X ˙ + a ˙ ( 0 ) ) + [ ( e / m ) A + ( e / m ) a ( 0 ) ⋅ ∇ A ] ⋅ ( X ˙ + a ˙ ( 0 ) ) − ε ,

which is regrouped and simplified to

L ≈ [ v ∥ b ( 0 ) + ( e / m ) A ] ⋅ X ˙ − ε + a ˙ ( 0 ) ⋅ [ ( e / m ) A + X ˙ ] + ( e / m ) a ( 0 ) ⋅ ( ∇ A ) ⋅ X ˙ + ( e / m ) a ( 0 ) ⋅ ( ∇ A ) ⋅ a ˙ ( 0 ) + a ˙ ( 0 ) 2 . (111)

The first terms in the above equation are independent on γ , the others should depend on γ even if the latest terms should be very little. Now, it is possible [

L ≈ [ v ∥ b ( 0 ) + ( e / m ) A ] ⋅ X ˙ + a ˙ ( 0 ) 2 / 2 − ε + d S / d t . (112)

as shown in [

Finally, defining the magnetic moment as

μ ≈ v ⊥ 2 2 | B | , (113)

then L g c = L − d S / d t is

L g c ≈ [ v ∥ b ( 0 ) + ( e / m ) A ] ⋅ X ˙ + ( m / e ) μ γ ˙ − ε , (114)

which is the lagrangian obtained in (106) if P ≈ v ∥ b ( 0 ) + ( e / m ) A ( t , X ) . At the same ordering, being the energy quadratic, the guiding center energy is E ≈ v ∥ 2 / 2 in such a way that the total energy is ε = E + ( m / e ) μ γ ˙ ≈ v ∥ 2 / 2 + μ | B | .

The guiding center coordinates in the presence of a magnetic field, similarly to the center of mass coordinates in a gravitational field, describe the origin of the reference frame where positions, velocities and time are efficiently measured, so that

x = X + ρ (γ)

u = U + ν (γ)

t = t b + τ ( γ ) .

It is worth noticing that the latter equation is often written in plasma physics as t = t slow + t fast ( γ ) , so dividing what depends on slow variations from what depends on fast variations. In the present analysis t b is considered as a reference time which it can also be used for obtaining the Abraham-Lorentz-Dirac force [

X ¨ ( t ) ≈ X ¨ ( t b ) + τ X ⃛ ( t b ) . (115)

^{2}The same definition pertains also to the gyrocenter when e.m. fluctuations are taken into account, see section VII.

It is worth to note that the guiding center transformation is simply a translational transformation on the extended phase space. All the coordinates are translated by a quantity depending on γ ∈ S 1 . This property allows the following new definition to emerge: the guiding center reference frame is the particular reference frame where the particle moves in a closed orbit with a periodic motion^{2}. The efficiency of describing the general motion is only because the orbit is reduced to a closed loop parametrized by the angle γ . In order to reach such reference system we must subtract the relativistic guiding center velocity U from u and also shift the position of the particle to the guiding center position X. In the guiding center reference frame it is possible to observe that the particle is gyrating in a closed loop with the cyclotron frequency.

If the manifold of the extended phase-space is not flat, then the above translations must be considered as if the quantities depending on γ are parallel transported over the manifold.

The coordinates z A with A = 0 , 1 , 2 , 3 , 4 , 5 , 6 , introduced in the previous section, belong to the extended phase space. As for general relativity, where a geometry is given to the space-time, in this section a geometry is given to the extended phase-space.

We have seen that in the presence of e.m. fields, it is useful to describe the motion in guiding center coordinates, z A = ( t , X , γ , μ , ε ) . For accuracy, the guiding center transformation is the map, T , that allows to describe particles through the guiding center coordinates, T : ( t , x , p ) → ( t , X , γ , μ , ε ) . It is worth noticing that the vector X indicates the position of the guiding center, not of the particle. If μ ≠ 0 then the particle is elsewhere from X.

The KK mechanism was used in the past to explain the presence of gravitation and electromagnetism thanks to the addition of, at least, a new coordinate of spacetime. The KK model can be obtained from a Hilbert-Einstein (HE) action extended to a space-time of five dimensions as reminded in the appendix. However, in the present approach, we adopt the same mechanism, in which the new dimension is a coordinate that belongs to the velocity space. In fact, the 5^{th} dimension is identified with the gyro-phase coordinate, γ . As a consequence we are changing the paradigm of the general relativity theory that only takes into account the space-time geometry. Thus, if you want to describe gravity then you can only consider the geometry of space-time, whilst if you want to describe gravity plus electromagnetism you have to consider the geometry of the extended phase space. Mathematically, it is not so difficult to extend the general relativity formalism to five or more (seven) dimensions. However, the physical interpretation of an Einstein equation in extended phase space, is quite unusual to be exposed in the present work. What is proposed here is a minimal change of the KK model and the use of the relativistic guiding center transformation. In this section we leave the Minkowski metric for a pseudo-Riemannian one.

Let’s start from the Poincaré-Cartan one-form in (84): L ^ d s ^ = − w A d z A , for A = 0 , 1 , 2 , 3 , 4 , 5 , 6 . The same one-form can be written as

L ^ d s ^ = − g ^ A B w B d z A , (116)

being L ^ a scalar quantity and where g ^ A B is the metric tensor with the property that w A ≡ g ^ A B w B . Thus, w B are the contravariant momenta. Once the metric tensor is appeared, it is possible to apply a variational principle for finding it. For this reason, we consider a lagrangian density over the extended phase space where the single particle lagrangian is multiplied for the distribution of masses and, then, added to the HE lagrangian in extended dimensions. In the following lagrangian density,

l a = f m L ^ − R ^ 16 π G ^ , (117)

f m is the scalar distribution function of masses, for simplicity only one species is considered; G ^ and R ^ are the gravitational constant and the scalar curvature for the extended phase space, respectively. The scalar curvature is defined as usual:

R ^ = g ^ A B R ^ i c A B , (118)

again, R ^ i c A B is the Ricci tensor in the extended phase space which is furnished of a Levi-Civita connection. The lagrangian, (117), is a lagrangian density over the extended phase-space and the action is computed from the integration of l a over the extended phase space. If | g ^ | indicates the square root of the absolute value of the determinant of the extended phase space metric, then the extended phase space volume element, d M , can be written as:

d M = | g ^ | d 7 z , (119)

if the guiding center coordinates are used then d 7 z = d t d 3 X d γ d ε d μ . Explicitly, the action is:

S = ∫ l a d M , (120)

which is a definite integration in a domain ∂ M of the extended phase space. It is possible to separate in l a the effects of different contributions. A matter lagrangian distribution:

l a m = − f m , (121)

a field lagrangian distribution:

l a f = − R ^ 16 π G ^ , (122)

and an interaction dynamics lagrangian distribution:

l a id = f m ( 1 + L ^ ) , (123)

^{3}We are implicitly imposing that matter cannot be created nor destroyed.

The distribution of masses, f m is taken as a scalar function: f m = f m ( z A ) ^{3}.

Within the guiding center description, f m indicates the presence of a particle of mass m with guiding center coordinates ( t , X , γ , μ , ε ) .

The particle described by f m must be counted only once to obtain the total mass, M, of the system. The following equivalence chain of integrations is assumed for the matter action, S m :

S m = − ∫ f m | g ^ | d 7 z = − ∫ ρ m − g d t d 3 X = − ∫ M d s ^ , (124)

where ρ m is the mass density and, above all, − g is the square root of minus the determinant of the space-time metric. In fact, if you call J P the quantity | g ^ | / − g , then:

ρ m = ∫ f m J P d γ d ε d μ . (125)

The density of masses is obtained from the integration of the distribution of masses in the velocity space. If you introduce unspecified velocities or momenta, P , with the only property that allows to write the latter velocity space volume element:

d 3 P = J P d γ d ε d μ , (126)

then the former integral is written in the usual form:

ρ m = ∫ f m d 3 P . (127)

Concerning the fields action, S f , we wish to have:

S f = − ∫ R ^ 16 π G ^ | g ^ | d 7 z = − ∫ F α β F α β 4 − g d t d 3 X − ∫ R 16 π G − g d t d 3 X , (128)

In order to obtain the latter result we will use the KK mechanism. However, before doing that, we are interested in studying the interaction dynamics action S id , that should be expressed by:

S id = ∫ f m ( 1 + L ^ ) | g ^ | d 7 z = − ∫ A α J α − g d t d 3 X , (129)

where J α is the charge four-current density which is a field depending on ( t , X ) . The former equation will be obtained in the forthcoming subsection. It is worth noticing that, if the above equations for l a m , l a f and for l a id , defined in (124), (128) and (129), respectively, are considered, once l a is integrated in the velocity space, then the following lagrangian density appears:

L = − ρ m − A α J α − F α β F α β 4 − R 16 π G . (130)

The latter is exactly the lagrangian density used for describing the presence of (e.m. interacting) matter as source of a gravitational field, which gives the Einstein equation, together with a charge four-current density as source of an e.m. field, which gives the Maxwell equations.

In lagrangian mechanics the symmetries of a system are expressed by the invariance of the lagrangian under the considered transformations. In relativity, the conservation of the energy-momentum tensor, T α β , is fundamental. The conservation of T α β is due to the symmetry of the lagrangian under the spacetime translation: X α → x α = X α + ρ α . This is also true if we explicitly take, X α = ( t b , X ) and ρ α = ( τ , ρ ) ; so that, x = X + ρ and t = t b + τ . If the manifold is not flat the translation is expressed by the parallel transport.

For our needs, the single particle lagrangian, L = p ⋅ u − ε γ v can be written with a null magnetic moment term: L = p ⋅ u − ε γ v + ( m / e ) μ 0 ω 0 , if μ 0 = 0 . Now, the guiding center transformation leaves unaltered the form of the lagrangian. In the non perturbative guiding center transformation, the momentum of the particle, p → P , becomes the guiding center momentum computed at the guiding center X and at the time t, whereas the particle relativistic velocity, u → U , becomes the relativistic guiding center velocity U. Moreover, the null magnetic moment μ 0 → μ becomes a positive magnetic moment so that the gyro-phase γ becomes meaningful (because if μ = 0 then γ is singular). The single particle lagrangian under such transformation is

L = p ⋅ u − ε γ v = p ⋅ u − ε γ v + ( m / e ) μ 0 ω 0 → L ^ = P ⋅ U − E U 0 + ( m / e ) μ γ ′ , (131)

which is the guiding center Lagrangian, already seen in the former section.

In the relativistic approach we haven’t yet considered a relation as ( m / e ) μ γ ˙ = ε − E , used for defining the frequency, γ ˙ . Such relation was used in the non relativistic case for obtaining p ⋅ v = P ⋅ V . In the relativistic case, another relation is chosen that allows to write L = − 1 + ( e / m ) u α A α ( t , x ) = L ^ with

L ^ = − 1 + ( e / m ) U α A α ( t , X ) , (132)

which is the same form of L. This means that u α A α ( t , x ) = U α A α ( t , X ) is preserved. From u α p α = U α P α + ( m / e ) μ γ ′ , it was immediately found that the required condition is reached if

( m / e ) μ γ ′ = 1 − U α U α . (133)

The latter relation is also more interesting if ( m / e ) μ γ ′ = U 4 U 4 , where U 4 = z 4 ′ = γ ′ and U 4 is firstly defined as U 4 ≡ w 4 = ( m / e ) μ . In such way that

U a U a = 1 , for a = 0 , 1 , 2 , 3 , 4. (134)

Moreover, if the relation w a = U a + ( e / m ) A a is used, then A 4 = 0 for consistency: there is not a 5^{th} component of the e.m. potential. The symmetry that leaves invariant the form of L = − 1 + ( e / m ) u α A α ( t , x ) = − 1 + ( e / m ) U α A α ( t , X ) is said misleading because there is no way, starting from the lagrangian (from dynamics), to distinguish particle’s coordinates from guiding center’s coordinates. The only chance for appreciating the difference is by measuring the dispersion relation: from kinematics, the particle has u α u α = 1 whilst the guiding center doesn’t, U α U α ≠ 1 . If we suppose to observe a helicoidal trajectory made by the motion of a charged particle in a given e.m. field, then such trajectory could be considered a solution of motion. However, it is possible to zoom on the trajectory, by increasing the sensibility of detectors, and discover that the simple helicoidal trajectory is made by another sub-helicoidal motion, as shown in the cartoon of

Moreover, such misinterpretation can be iterated (with some constrains e.g. the velocity cannot overcome the speed of light), so that the sub-helicoidal motion can, once again, hide another subsub-helicoidal motion at a finer scale. Similarly to a fractal, when the magnetic field differs from being constant and uniform a family of solutions enriches the extended phase space of helicoidal trajectories made by other helicoidal trajectories. It is worth noticing that realistic magnetic fields are never constant and uniform and, moreover, any realistic detector doesn’t have infinite resolution.

The approximation of considering the guiding center motion instead of the

particle motion is said drift approximation and, if applied with criteria, it becomes the zero-th order approximation in all the gyro-kinetic codes used for studying magnetic confined plasmas for controlled fusion through a kinetic perspective.

It is worth noticing that there is another interpretation where many trajectories are described by the same motion of a representative guiding center. The latter interpretation is possible because we have considered all the trajectories with free initial and final conditions in the variational approach in Section II. In fact, if we impose with (almost) certainty the initial and the final values of the particle’s coordinates then there is only (almost) a unique solution of motion, whilst for an initial and final uncertainty, there is the possibility to have many trajectories that differs by the value of the magnetic moment and by the initial value of the gyrophase. Thus, the question is: “what are the trajectories that minimize the action and are also well represented by the Lorentz’s force law?”, instead of being “what is the trajectory that minimizes the action and is solution of the Lorentz’s force law?”. Those trajectories are indistinguishable and can be resolved only after a measurement, like for the collapse of a quantum state into a physical eigenstate in quantum mechanics. Indeed, the only way for distinguishing a guiding center from a particle is from the misleading condition in (134) that pertains to kinematics, being expressed by the Lorentz violation, U α U α ≠ 1 . The dynamics is still preserved by the same lagrangian.

Thanks to the misleading condition, Equation (134), it is very easy to show that the action S id takes the desired form (129) when the guiding center coordinates are used. In fact, L ^ = − 1 + ( e / m ) A α U α and

S id = ∫ f m ( 1 + L ^ ) | g ^ | d 7 z = − e m ∫ ρ m A α U ¯ α − g d t d 3 X . (135)

If J α = ( e / m ) ρ m U ¯ α , being

ρ m U ¯ α = ∫ f m U α d 3 P , (136)

then the former is exactly the relation in (129).

We have just seen that the guiding center transformation, which is a particular local translation in the extended phase space, is a symmetry because it leaves the same lagrangian form. In analogy to what happens for the local translation in spacetime, the conserved quantity for the present symmetry should be called the extended energy-momentum tensor T ^ A B , which is obtained from the variation of l a m + l a id = f m L ^ with respect to the metric tensor variation, δ g ^ A B :

T ^ A B δ g ^ A B = − 2 δ ( l a m + l a id ) + g ^ A B ( l a m + l a id ) δ g ^ A B . (137)

Now, the Einstein tensor for the extended phase space is obtained from the variation of l a f with respcet to δ g ^ A B :

G ^ A B = R ^ i c A B − R ^ g ^ A B / 2 , (138)

and the Einstein equation can be written also for the extended phase space,

G ^ A B = 8 π G ^ T ^ A B . (139)

It is worth noticing that, if confirmed, we have just obtained gravitation and electromagnetism from a geometrical perspective. A similar equation holds in the Projective Unified Theories proposed by Schmutzer [

However, when extending the dimensionality from four to seven it is possible to take into account many possibilities. We will show that the abelian nature of the gauge theory comes suddenly from the choice of the γ ∈ S 1 gyro-phase as coordinate of the velocity space but, anyways, the gauge theory could become non abelian by choosing other variables with different groupal properties from the gyrophase. The possibility to definitely separate in the extended phase space what belongs to spacetime and what to velocity space must be reformulated. It seems that the space-time is simply defined as the domain of variation of the e.m. fields, in such a way that we need an e.m. field for defining space-time variables. Such route needs some care and it cannot be taken just now. We prefer to show the minimal five dimensional extension of gravitation explicitly using the guiding center coordinates. Such extension is sufficient to include electromagnetism. Moreover, the present description is facilitated by the work of KK, because most of the general relativity equations that we will soon encounter, have already been studied [

Instead of deriving the metric tensor from a variational approach, it is possible to settle the metric tensor directly. This can be less elegant but easier to do mostly because it has already been done. The original KK mechanism needs an extension of the dimensionality of space-time by only one dimension. Only five dimensions occur to display electromagnetism and gravitation. However, we have formulated an extension to seven, not five, dimensions of general relativity. This is too general for the present scope, but we have seen that in the single particle one-form (83) there is only the variation of five coordinates: z a = ( t , X , γ ) , with a world line coordinate s ˜ = s ˜ ( z a ) , for a = 0 , 1 , 2 , 3 , 4 . In this subsection we re-formulate the lagrangian density, (117), in five dimensions and, after adopting the KK metric tensor, we prove the Equation (128), which is the last equation needed to get the wanted lagrangian density (130).

The KK mechanism is used following the review articles [

L ˜ = − g ˜ a b w a z ′ b , for a , b = 0 , 1 , 2 , 3 , 4 . (140)

Also the lagrangian distribution, (117) can be considered into five dimensions:

l a = f m L ˜ − R ˜ 16 π G ˜ , (141)

being R ˜ the five dimensional scalar curvature, and G ˜ the five dimensional gravitational constant. In practice, R ˜ / G ˜ = R ^ / G ^ , as if we are considering flat the space described by the canonical coordinates ε and μ . It is worth noticing that although in five dimensions, all the quantities can depend also on ε and μ , e.g the distribution function f m is always the distribution of masses in the whole extended phase space and it surely depends on ε and/or μ if it describes an equilibrium [

S = ∫ l a | g ˜ | J ˜ P d t d 3 X d γ d ε d μ . (142)

Finally, we use the following KK metric tensor:

g ˜ a b = | g α β + κ 2 φ 2 A α A β κ φ 2 A α κ φ 2 A β φ 2 | . (143)

If the chosen signature is η α β = diag ( + 1, − 1, − 1, − 1 ) then φ 2 < 0 . Differently from KK, setting κ 2 φ 2 = − k G 2 and φ 2 = − k G 2 ( m / e ) 4 μ 2 (or κ μ = ( e / m ) 2 ), the metric tensor becomes:

g ˜ a b = | g α β − k G 2 A α A β − k G 2 ( m / e ) 2 μ A α − k G 2 ( m / e ) 2 μ A β − k G 2 ( m / e ) 4 μ 2 | . (144)

being k G a constant that will be specified below. From (208), it is possible to obtain the contravariant momenta.

w a = g ˜ a b w b = | U α ( e / m ) ( 1 / μ ) [ 1 + ( e / m ) 2 ( 1 / k G ) 2 + L ˜ ] | , (145)

in such a way that, from L ˜ = − w a U a , it is obtained the constancy of L ˜ in terms of important physical constants:

L ˜ = − 1 − 1 2 k G 2 ( m / e ) 2 . (146)

The latter metric tensor is used to compute the five dimensional scalar Ricci tensor (221): R ˜ = R − κ 2 φ 2 F α β F α β / 4 . Now, the field action is

S f = − 1 16 π G ˜ ∫ d t d 3 X | g ˜ | ( R + k G 2 4 F α β F α β ) J ˜ P d γ d ε d μ , (147)

where | g ˜ | is | g ˜ | = − g ( m / e ) 2 k G μ . For obtaining the standard gravitational plus e.m. fields action, k G must be k G 2 = 16 π G , so that

G ˜ = G ∫ ( m / e ) 2 k G μ J ˜ P d γ d ε d μ . (148)

and

S f = − ∫ − g d t d 3 X R 16 π G − ∫ − g d t d 3 X F α β F α β 4 . (149)

It is worth to note that the single particle interaction density lagrangian comes to be:

L ˜ ime = − e 2 32 π m 2 G = − α fs 32 π λ c 2 l p 2 . (150)

where α fs = e 2 / ℏ , λ c = ℏ / m and l p = ℏ G .

In this way, we have obtained the lagrangian density in (130) from the five dimensional lagrangian (141). It is worth noticing that, even if the terms in the lagrangian density (130) are the desired ones, they are referring to fields on ( t , X ) where X is the guiding center position and it doesn’t indicate the position of a particle. This is an effect of the misleading symmetry. The problem is that once we have integrated the lagrangian density, expressed in guiding center coordinates, on the velocity space, we have lost the possibility to know where the particles effectively are. This means that the present theory is non local. Fortunately, such non-locality helps for the consistency of electrodynamics, e.g. the problem of self-energy, or self-interaction, is promptly solved once a non-locality property is assumed. Moreover, we already know that, at some scale, an indetermination principle should be invoked. The relation between the misleading symmetry and the quantum non-locality property should be investigated. A simple guess is the following. In the Bhomian formulation [

The KK mechanism was discarded as a possible true mechanism of Nature because it holds many problems. The standard doubts refer to the reason for applying the cylinder condition, which is at the origin for explaining compactification. Another problem is the compactified scale length of the order of the Planck length, l p . Such scale length is inconsistent with the observed masses of elementary particles. Other approaches without these two ingredients, compactification and cylinder condition, are commonly less considered. However, all the problems are inherited to explain why the fifth dimension is unobservable [^{th} dimension belonging to the velocity space should set the length scale of the extra dimension equal to the Compton length, not to the Planck length. Immediately, it is recognized that with the present, now compactified, KK mechanism, also the scale of masses assumes the correct value. With an indetermination principle, the extra-dimension scale length becomes important because it is not possible anymore to know, at the same time, both the position and the velocity of the particle. Within quantum mechanics, it becomes forbidden to observe a gyro-radius below of the order of the Compton length.

The extension of the present theory to quantum mechanics will be described in another work which is in preparation. However, here it can be roughly shown how the present approach is not too much in conflict with quantum mechanics, thanks to the misleading symmetry and the instability of the guiding centers due to electromagnetic fluctuations.

In this section we introduce quantum rules without following the orthodox way. The probabilistic concepts that pertain to the quantum world are shown to be consequences of e.m. fluctuations. Several studies concerning the relation of quantum mechanics and stochastic processes are described in books like [

The e.m. fluctuations are commonly considered separately from the guiding center description. There is a simple reason for this, indeed in non relativistic regime, it is possible to separately take into account the time behavior of the e.m. fields. In plasma physics applied to laboratory plasmas this is almost the case, because the guiding center approach is used for describing particles motion in the background equilibrium e.m. fields ( E 0 , B 0 ) that don’t explicitly depend on time. The effective e.m. fields will be affected by changes induced by a redistributions of charges in the plasma. Such changes are e.m. fluctuations and they are particularly difficult to model because they are caused by collectives phenomena. However, in plasma physics modeling, the current approach [

L = x ˙ 2 / 2 + ( e / m ) A 0 ( t , x ) ⋅ x ˙ − ( e / m ) Φ 0 ( t , x ) + ( e / m ) δ ξ A ⋅ x ˙ − ( e / m ) δ ξ Φ ,

where A 0 α = ( Φ 0 , A 0 ) is the (deterministic) four-vector potential and δ ξ A α = ( δ ξ Φ , δ ξ A ) is the stochastic four-vector potential fluctuations. The e.m. fluctuating fields could be written as δ ξ E = − ∂ t δ ξ A − ∇ δ ξ Φ and δ ξ B = ∇ × δ ξ A , but some care should be considered when applying the stochastic differential calculus on such stochastic quantities.

The gyrocenter description is easily obtained from the guiding center description, because the effects of fluctuations will be easily reflected on the guiding center transformations that become

X ¯ = X + ξ , (151)

where X ¯ is the gyro-center position, X is the guiding center position and ξ is the guiding center displacement. Similarly for the velocity,

V ¯ = V + δ ξ V , (152)

where V ¯ is the gyro-center velocity, V is the guiding center velocity and δ ξ V = ξ ˙ is the guiding center velocity displacement. Concerning stochastic processes, it is better to write the latter equation with the increments instead of the derivatives:

d X ¯ = V d t + d ξ . (153)

Moreover, being V = v − σ , the gyro-center increment d X ¯ is rewritten as

d X ¯ = ( v − σ ) d t + d ξ , (154)

where the guiding center velocity, V, is the mean gyro-center velocity, and d ξ at time t is independent of X ¯ for a time before t. In stochastic differential calculus the limit d t → 0 should be considered with care and it is meaningful to define two kinds of derivatives. The forward derivative:

D X ¯ = lim d t → 0 + 〈 X ¯ ( t + d t ) − X ¯ ( t ) d t 〉 , (155)

and the backward derivative

D ⋆ X ¯ = lim d t → 0 − 〈 X ¯ ( t ) − X ¯ ( t − d t ) d t 〉 , (156)

Here, D X ¯ = V and D ⋆ X ¯ = V ⋆ . In such a way that they are coincident, V = V ⋆ , when X ¯ is differentiable. Thus, the stochastic process should be characterized also by the backward increments that can be written as

d X ¯ = V ⋆ d t + d ξ ⋆ , (157)

where d ξ ⋆ at time t is independent of X ¯ for a time after t. In general, V ⋆ = v − σ ⋆ . Finally, the stochastic process ξ is considered identical to ξ ⋆ and a simple Wiener process with

〈 d ξ 〉 = 〈 d ξ ⋆ 〉 = 0 , (158)

and

〈 d ξ i d ξ ⋆ j 〉 = 2 ν p δ i j d t , (159)

with d ξ i and d ξ ⋆ j specifying the cartesian components of the stochastic vectors d ξ and d ξ ⋆ , respectively. The constant ν p indicates the product of a length times a velocity and coincides with the diffusion coefficient of the stochastic process. It is worth noticing that the origin of such diffusive process is due to the e.m. fluctuations. The implicit reason for such fluctuations are the absorbed and/or emitted radiation by the charge, its motion becomes markovian, as for the brownian particle. If we can ruled out the radiation, then the behavior could be different, for instance ν p = 0 . However, here we will always consider the presence of an e.m. field and, at least, one charge. The dynamics of a charge cannot correctly be described if separated from the e.m. field, that implies ν p ≠ 0 .

It is possible to associate two Fokker-Planck (FP) equations to the stochastic process. For a probability density function, f, the forward FP equation is:

∂ t f = − ∇ ⋅ ( V f ) + ν p Δ f , (160)

or

∂ t f + V ⋅ ∇ f = − f ∇ ⋅ V + ν p Δ f . (161)

Similarly, the Fokker-Planck equation for the backward process is

∂ t f = − ∇ ⋅ ( V ⋆ f ) − ν p Δ f , (162)

or

∂ t f + V ⋆ ⋅ ∇ f = − f ∇ ⋅ V ⋆ + ν p Δ f . (163)

From the sum of the two Fokker-Planck equations,

∂ t f = − ∇ ⋅ ( f V + V ⋆ 2 ) . (164)

From subtracting the two FP equations,

∇ ⋅ ( f σ − σ ⋆ 2 ) + ν p Δ f = 0. (165)

From the latter, Nelson argued the following particular solution for σ − σ ⋆ = 2 u N , where the osmotic velocity is

u N = − ν p ∇ l o g f , (166)

as in [

v N = V + u N . (167)

The current velocity is the gyro-center velocity when ξ ˙ is replaced by u N . Obviously, when fluctuations are neglected, the gyro-center velocity becomes the guiding center velocity.

If the backward process is realized with V ⋆ = v N + u N , then the continuity equation, from Equation (164), is

∂ t f = − ∇ ⋅ ( f v N ) , (168)

This is the reason for appropriately calling the gyro-center velocity, v N , as the current velocity.

In a straight and uniform magnetic field, we have seen that σ = v ⊥ , which can be opportunely written as σ = − ρ L ω c ( e 1 s i n γ + e 2 c o s γ ) = ρ L 2 ω c ∇ γ , if no fluctuations are considered. Here, γ is always the gyro-phase, with ∇ γ = e γ / ρ L , and ω c = ( e / m ) | B | . For such case without fluctuations, ∇ f = 0 , or f = 1 , ensuring determinism. Thus, by introducing fluctuations that modify the effective velocity of the charge, v, and the velocity σ. In such way that v = v N + σ − u N = V + σ . It is worth noticing that he velocity v is an effective velocity, which is very useful because both the true velocity and the true e.m. field acting on the charge are unknown. Fluctuations add a term, the osmotic velocity u N , to σ that becomes:

σ = − ν p ∇ l o g f + ρ 2 ω c ∇ γ , (169)

where the Larmor radius is not anymore constant and it has been substituted with the gyroradius ρ L → | ρ | . Thus, v = v N + ρ 2 ω c ∇ γ . The backward velocity, − σ ⋆ is obtained changing the direction of γ (or the sign of the charge): − σ ⋆ = − ν p ∇ l o g f − ρ 2 ω c ∇ γ . In such a way that σ + σ ⋆ = 2 ρ 2 ω c ∇ γ . Always in the straight and uniform equilibrium magnetic field case, by taking f ∝ 1 / ( π ρ 2 ) , that means that the probability for finding the particle is, roughly, inversely proportional to the area of the disc of radius | ρ | ^{4}. Now, the divergency of ∇ ⋅ [ f ( σ + σ ⋆ ) ] = 0 , being γ an angle so that ∇ 2 γ = 0 . In such case the continuity equation reads

∂ t f = − ∇ ⋅ ( f v ) , (170)

^{4}Another, more general, choice is f − 1 ∝ π n ρ 2 n / Γ ( n / 2 + 1 ) , which is the volume of a n-ball, with n ∈ ℕ .

being ∇ ⋅ [ f ( V + V ⋆ ) ] = 2 ∇ ⋅ ( f v ) − ∇ ⋅ [ f ( σ + σ ⋆ ) ] = 2 ∇ ⋅ ( f v ) . The gyro-velocity,

σ = 2 ν p | ρ | e ρ + | ρ | ω c e γ , (171)

is maintained perpendicular to the equilibrium magnetic field. The product ρ ⋅ σ = 2 ν p is constant, so that if the radius of the disc, | ρ | , increases (e.g. absoption of radiation) then the radial velocity decreases. Thanks to the gyrating part, the overall velocity, | σ | , increases. On the contrary, if | ρ | decreases (e.g. emission of radiation), the gyrating part of σ becomes negligible with respect to the radial velocity that explodes as ~ 1 / | ρ | . Such remarks, even if obtained in a non relativistic treatment, allows to roughly deduce the order of magnitude of the constant ν p if a minimum value of | ρ | and, correspondingly, a maximum velocity is conceived. Let’s indicate the minimum radius, corresponding to the diffusion length, with λ c , then a maximum velocity is obtained and indicated with c ≈ 2 ν p / λ c .

The gyro-phase symmetry of the system is maintained so that the magnetic momentum is conserved, from Equation (62):

μ = ( e / m ) σ 2 2 ω c = ( e / m ) ω c ρ 2 2 + 2 ( e / m ) ν p 2 ρ 2 ω c , (172)

where the contribution of fluctuations with respect to the standard magnetic momentum is evident from the appearance of the factor ν p in the second term on the right hand side. As for the gyrating velocity, also the magnetic moment is never vanishing in the presence of fluctuations. Finally, the energy per unit mass is

ε = v ∥ 2 2 + ω c 2 ρ 2 2 + 2 ν p 2 ρ 2 (173)

with a zero field point energy per unit mass [

ε zpf ≈ ( λ c 2 ω c 2 + c 2 2 ω c ) ω c . (174)

Thus, μ B = ( e / m ) ( λ c 2 ω c 2 + c 2 ) / ( 4 ω c ) . Finally, the prestige is the following, if λ c 2 ω c 2 = c 2 then the minimum energy of the charge (times the mass) is E zfp ≈ m c 2 . The surprise is that instead of being the energy of the particle at rest, in the present case, it is the guiding center which is at rest. Above all, the energy m c 2 has been obtained without a relativistic approach, but with a magnetic field | B | = ( m / | e | ) ( c / λ c ) . This is not the only surprise, indeed, if ν p = ℏ / ( 2 m ) (as in [

ρ ⋅ ( m σ ) = ℏ , (175)

If you introduce Δ x = | Δ x | e ρ , with | Δ x | ≥ | ρ | and Δ p = | Δ p | σ / | σ | with | Δ p | ≥ | σ | , as representative estimators of the indetermination of the position and of the velocity, respectively, of the charge with respect to the gyro-center, then

Δ x ⋅ Δ p ≥ ℏ (176)

which is similar to the Heisenberg indetermination principle. The explanation, with respect to the Copenhagen interpretation, is quite different. The charge is moving with a newtonian deterministic motion, the gyro-center is moving with a stochastic motion and, due to such stochasticity, it is not allowed to know exactly the position and the velocity of the gyrocenter with respect to the charge and/or viceversa. Within the limit imposed by the indetermination principle the gyrocenter and the charge are undistinguishable entities. In the following, the appellation of elementary particle will be shown to be better suited for the stochastic gyro-center than for the charge.

The zero field point energy (times the mass) becomes

E zfp ≈ ℏ ω c , (177)

about twice w.r.t. the one obtained from a quantum oscillator, but what is exactly needed for obtaining the black-body spectrum from the Planck distribution. Moreover, with the latter z.f.p. energy, the energy of the charge, E 2 = m ε , with respect to the energy of the guiding center, E 1 = m v ∥ 2 / 2 , is: E 2 − E 1 = ℏ ω c . The former is similar to the Bohr’s frequency relation, but it is a consequence of Equation (60) when ( m / | e | ) μ = ℏ / m . It is worth noticing that such results have been obtained without introducing quantum mechanics or special relativity issues.

It is worth noticing that the non vanishing magnetic moment, due to the e.m. fluctuation is estimated to μ B = ( | e | / m 2 ) ℏ / 2 which is the Bohr magneton. Moreover, asking for f to be inversely proportional to the disc with radius equal to the radial position of the charge, we are constructing a measure for determining the probability of finding the unknown position of the particle. Is it possible that such construction leave us close to the Born interpretation?

An interesting behavior is seen if the canonical magnetic field line is closed. In the present paragraph we analyze the behavior of a charge when the canonical magnetic field is closed into a circle with radius a B = λ c / α fs ≫ λ c . In the next paragraph, we will consider a system of an electron and an ion when the canonical magnetic field is closed into an invariant tori. It is worth to note that it is important to have, at least, α fs − 1 = O ( 10 2 ) for closing the circle without changing too much the former considerations obtained with the straight magnetic field case. In fact, for a charge moving on a circle with a small radius, λ c , the magnetic field is still sufficiently straight and uniform even if the field line is closed in a circle of radius O ( 10 2 ) bigger than λ c . A charge moving circularly with a radius λ c and velocity λ c ω c , gives rise to a magnetic field which is almost straight in the vicinity of the charge but that it closes in a circle when the effects of the charge are mostly reduced. If ω c = c / λ c then the radius of the magnetic field line passing close to the center of the circle, and for which the motion of the charge is mostly the same as if it would straight, is λ c / α fs .

Thus, let’s take v ∥ → V b = a B θ ˙ , where θ is a poloidal angle. Now, the charge is moving with an orbit on the surface of a torus of radius a B and described by the two angles, γ and θ . The orbit is closed e.g. if, given n ∈ ℕ then n θ ˙ = ω c . The closure can also happen on other tori with a radius greater then a B ; such tori where the orbit are closed loops are called invariant tori. It is worth noticing the appearance of a diophantine relation. Moreover, if both the velocity of the charge in the Larmor circle and of the guiding center in the poloidal circle is c, then α fs = 1 / n is the inverse of an integer. The former picture is an approximation because the effects occurring when the cylinder is closed onto a tori has not been properly taken into account.

A picture very close to the de Broglie’s model but with a reasoning applied to an invariant tori on a 3D space, instead to a simple closed string on a 2D surface, is suggested, here, once the system made by an electron with mass m e , and an ion with mass m A and charge Z | e | is considered. Such analysis is done for considering a rough relation between the toroidal magnetic configuration, as seen in tokamaks, and some aspects of the Bohr atomic model. Only in the following section, a rigorous non relativistic atomic model can be addressed by deriving Schrödinger equation. However, a suggestive idea explaining some old disputes on the first appearances of quantum behaviors, is shown (without quantum mechanics). In the presence of an axisymmetric magnetic field, described by (41), the guiding center of the electron is given by Equation (42):

V e = λ e m e ∇ P ϕ × ∇ ϕ + e m e ( P ϕ − ψ p ) ∇ ϕ , (178)

being λ = − ψ p / F . If P ϕ = ψ p + λ F then the former velocity can be rewritten as

V e = e m e P ϕ − ψ p F ( ∇ P ϕ × ∇ ϕ + F ∇ ϕ ) . (179)

In parenthesis the magnetic field B c = ∇ P ϕ × ∇ ϕ + F ∇ ϕ is rewritten with the Clebsh representation as:

B c = ∇ P ϕ × ∇ ( ϕ − q sf θ ) , (180)

where θ is the generalized poloidal angle and

q sf = B c ⋅ ∇ θ B c ⋅ ∇ ϕ (181)

is the safety factor. Now, P ϕ is the poloidal magnetic flux of B c . It is possible to introduce a flux radial coordinate, r, in such a way that P ϕ ∝ r 2 , which means that we are considering nested poloidal surfaces with circular cross sections. We also consider the presence of a positive charge, Z | e | , which is moving toroidally with the same toroidal component of the electron guiding center velocity, For describing the effective velocity of the electron, as for the ion, we should add to the guiding center velocity also the gyro-velocity, σ, with the osmotic velocity. However, we only wish to consider a particular case that reminds the old but always fascinating Bohr’s atom model. It is chosen a very strange (never seen in tokamaks) safety factor with the following dependency on r:

q sf = r / a B , with q sf ≥ 1 . (182)

Thus, when the canonical magnetic field lines are closed (the guiding center orbits are closed, too), the resonant magnetic flux surfaces, P ϕ . res , are determined by the condition r / a B = n ∈ ℕ , or:

r = n 2 a B , (183)

in such way that P ϕ . res ∝ n 4 .

Thus, only for some diophantine values of r the guiding centers are resonants. Here, the question is if the magnetic field that allows the guiding center of the electron to move on invariant tori can, or cannot, be generated by the same electron and ion that we are describing. It is not easy to answer but what it can be said is that if it is chosen the reference frame where the toroidal guiding center velocity of the electron is null, then we arrive at the simple description of an electron moving circularly around a positive ion. In such reference frame, the ion is fixed. Concerning the electron, its motion is due to the cylindrical symmetry of the system and to the electric field generated by the central positive ion. The balance of the electric field with the centripetal motion is

Z e 2 r 2 = m e r θ ˙ 2 , (184)

which means

θ ˙ = Z e 2 m e r 3 = 1 n 3 Z e 2 m e a B 3 . (185)

The angular momentum, L ϕ = m e r 2 θ ˙ is proportional to the number of poloidal cycles, n, that are necessary to close the orbit in the tori:

L ϕ = n m e Z e 2 a B . (186)

Finally, if a B = ℏ 2 / ( m e Z e 2 ) is the Bohr's radius, then the angular momentum is quantized:

L ϕ = n ℏ , (187)

which is the Bohr-Sommerfield rule.

Even if the former examples are somehow suggestives, the analysis is too rough and inappropriate for the delicateness of the problem. In the next section we abandon those simple cases for addressing a correspondence between stochastic gyrokinetic and quantum mechanics.

Finally, the acceleration of the gyro-center is considered as in [

a N = D D ⋆ + D ⋆ D 2 X ¯ . (188)

There are other possibilities on defining an acceleration but in this work they are not taken into account. Once the derivative is applied to D X ¯ = V and D ⋆ X ¯ = V ⋆ , we find the Nelson’s acceleration:

a N = ∂ t v N + v N ⋅ ∇ v N − u N ⋅ ∇ u N + ν p ∇ 2 u N , (189)

It is worth noticing that v ˙ N ≠ a N , if fluctuations are considered. In other words, the trajectory of a particle is different if f ≠ 1 and ν p ≠ 0 . The idea of Nelson was to associate such discrepancy, that depends on the presence of fluctuations, with the quantum mechanical formulation.

In our case a N = ( e / m ) ( E + v N × B ) and, with the same procedure described in section II, it is possible to arrive at a modified velocity law equation:

∂ t p N + ∇ ε N − v N × ∇ × p N = ( ν p 2 / 2 ) ∇ ( ∇ l o g f ) 2 + ν p 2 ∇ ∇ 2 l o g f ,

being p N = v N + ( e / m ) A and ε N = v N 2 / 2 + ( e / m ) Φ . However, a simple transversal electric field, E t = − ( m / e ) ∂ t p N − ( m / e ) ∇ ε p , is obtained if

ε p = v N 2 / 2 + ( e / m ) Φ − ( ν p 2 / 2 ) ( ∇ log f ) 2 − ν p 2 ∇ 2 log f , (190)

then

E t + v N × B c = 0 , (191)

similarly to the Lorentz’s force law case. It is worth noticing that the relation between ε p and the Bohm quantum potential [

Q B = − ν p 2 f − 1 ∇ 2 f = ν p ∇ ⋅ u N − u N 2 , (192)

is

ε p = ε N + u N 2 / 2 + Q B .

Now, by considering the gyrating particle solution with B c = 0 , it means that p N is a gradient, which is written p N = ∇ S N and E t = 0 . For simplicity, let’s take

ε p = − ∂ t S N . (193)

Nelson has shown in [

ψ = f e − i γ , (194)

where γ = S N / ( 2 ν p ) is always the gyrophase, and being an angle it is multivalued as noticed by Wallstrom. It is worth noticing that the gyrating particle solution corresponds to the zitter-solution already described in section III (3.1). In fact, it has been recently noticed in [

f ∂ t γ = i ψ ∂ t ψ ⋆ − ψ ⋆ ∂ t ψ 2 , (195)

f ∇ γ = i ψ ∇ ψ ⋆ − ψ ⋆ ∇ ψ 2 , (196)

and

f ∂ t log f = ∂ t f = ψ ⋆ ∂ t ψ + ψ ∂ t ψ ⋆ (197)

f ∇ log f = ∇ f = ψ ⋆ ∇ ψ + ψ ∇ ψ ⋆ . (198)

Thus,

u N = − ν p ψ ⋆ ∇ ψ + ψ ∇ ψ ⋆ ψ ⋆ ψ (199)

and the stochastic gyrocenter velocity, v N = − 2 ν p ∇ γ − ( e / m ) A , is

v N = + i ν p ψ ∇ ψ ⋆ − ψ ⋆ ∇ ψ ψ ⋆ ψ − ( e / m ) A . (200)

At the moment it doesn’t occur to specify that the potentials are computed in X ¯ , however it makes a certain difference.

The Schrödinger Equation from Classical Physics and StochasticityEven if Nelson was clear in his derivation, we follow a different approach, a constructive one, to reach the Schrödinger equation. It is here required that v N ⋅ u N = 0 , which means that the stochastic gyrocenter velocity is perpendicular to the osmotic velocity due to fluctuations. Such choice is a requirement on f. From the guiding center velocity, V = v N − u N , it follows that V 2 = v N 2 + u N 2 = ( v N + i u N ) ⋅ ( v N − i u N ) . In terms of ψ and ψ ⋆ , V 2 is below computed. Firstly

v N − i u N = ψ ⋆ − 2 i ν p ∇ − ( e / m ) A f ψ , (201)

and

v N + i u N = ψ 2 i ν p ∇ − ( e / m ) A f ψ ⋆ . (202)

Thus, the guiding center velocity squared is

V 2 = f − 1 [ 2 i ν p ∇ − ( e / m ) A ] ψ ⋆ ⋅ [ − 2 i ν p ∇ − ( e / m ) A ] ψ = 2 i ν p f − 1 ∇ ⋅ f ( v N + i u N ) + ψ ⋆ f − 1 [ − 2 i ν p ∇ − ( e / m ) A ] 2 ψ .

From the continuity Equation (170) and from the Bohm’s quantum potential (192), V 2 / 2 is rewritten as

V 2 2 = − i ν p f − 1 ∂ t f − Q B + ψ ⋆ f − 1 [ − 2 i ν p ∇ − ( e / m ) A ] 2 2 ψ (203)

Finally, it occurs only set all the pieces together, from (190):

ε p = V 2 / 2 + ( e / m ) Φ + Q B = − i ν p f − 1 ∂ t f + ψ ⋆ f − 1 [ − 2 i ν p ∇ − ( e / m ) A ] 2 2 ψ + ( e / m ) Φ , (204)

being Φ computed at the gyrocenter position, X ¯ . Moreover, being ε p = − 2 ν p ∂ t γ , the following equation is easily obtained:

− 2 ν p ∂ t γ + i ν p f − 1 ∂ t f = ψ ⋆ f − 1 [ − 2 i ν p ∇ − ( e / m ) A ] 2 2 ψ + ( e / m ) Φ .

If ν p = ℏ / ( 2 m ) , as already considered in the straight and uniform magnetic field case with fluctuations, then the Schrödinger equation is derived:

2 i ν p ∂ t ψ = [ − 2 i ν p ∇ − ( e / m ) A ] 2 2 ψ + ( e / m ) Φ ψ . (205)

Finally, if we set the minimum allowed magnetic moment to

μ = − ( e / m ) ν p = μ B , (206)

then the order of magnitude of the compactification scale in the KK mechanism is the Compton length, λ c , ensuring the correct mass scale for the elementary particles. Moreover, ν p is the diffusion coefficient in (159), in such a way that the Wiener process is recognized to be universal (as already noticed by Nelson).

The non-perturbative guiding center transformation has been extended to the relativistic energies. Within the relativistic regime, the same Equation (8) already seen in the non relativistic treatment [

Some important solutions of the velocity law are considered in Section III. Here, the difference between the guiding particle solution in gyrokinetic-like ordering, in MHD-like ordering, and the gyrating particle solution, is shown. All these solutions are practically identical to the non-relativistic case, which have been analyzed in detail in [

Furthermore, a general relativity approach for describing electromagnetism using the relativistic guiding center transformation is suggested. It is shown that the formalism of non-canonical hamiltonian mechanics is what is needed to extend the presence of electromagnetic dynamics to the general relativity formalism. An Einstein’s Equation (139), for the extended phase space can be settled for describing both the interactions: elelctromagnetism plus gravitation. Moreover, it has been proved that, for the guiding center coordinates, the relevant dynamics are five dimensional as for the original KK mechanism. The lagrangian density (130), which is used for describing both gravitation and electromagnetism, has been obtained. The metric tensor has been explicitly written in (144). The gyro-phase coordinate, γ , is proposed to be the fifth KK coordinate. Thus, the extra-dimension is not an unobservable spacetime dimension but a measurable coordinate of the velocity space used for describing motion on the extended phase space. For this reason, the KK mechanism does’t need a compactification procedure, anymore. If γ ∈ S 1 , which is exactly obtained only for the non-perturbative guiding center transformation, an abelian gauge theory can be settled: electromagnetism is served on the gravitational banquet. The novelty of the present work relies on the fact that the geometry of the velocity space must be taken into account also for describing the same gravitational field acting on the particles.

In the last section, some speculative possibilities are taken into account. Once electromagnetic fluctuations are considered, it is not allowed anymore to shrink the gyroradius to zero. From the guiding center transformation to the stochastic gyrocenter one, it occurs to radically change the velocity law, which means that the gyrocenter moves differently with respect to the guiding center. Using Nelson’s approach to quantum mechanics, answering to the Wallstrom’s criticism and giving a physical justification to the fluctuations required by Nelson’s approach, then it has been shown how to derive the Schrödinger Equation (205), with all its implications.

Finally, considering the diffusion coefficient as proportional to the Planck constant and inversely proportional to the inertial mass, it has been shown that the scale of length for the extra dimension is the Compton length, instead of the Planck length. This is correct also from another kind of consideration. Thus, if the extra dimension belongs to the velocity space, the Heisenberg indetermination principle which forbids the contemporary knowledge of position and of velocity of the particle, led to a different scale length limitation, which is caused by the incommensurability between velocities and positions instead of by the unobservability of the 5th dimension. Thus, the length scale for the new compactification scheme is fixed by the Compton length, ensuring the correspondence with the observed masses.

What emerges from such picture is that some quantum effects can be also explained, and not only interpreted, by the old classical mechanics. Once the non perturbative guiding center and the stochastic gyrocenter transformations are applied to plasma physics then a field theory (on extended phase-space) approach can be, finally, well suited for solving nonlinearities. From the plasma lagrangian density in (2) where “something new” is substituted with the Hilbert-Einstein term on extended phase-space, the consequences and the differences with the standard formulation should be investigated. Once macro- and micro-behaviors will be described in a unified manner, then the multi-scale non-linear problem encountered in tokamak physics can be reformulated with new tools; also for this reason, the non-perturbative guiding center and the stochastic gyrocenter transformations have been proposed.

The author wishes to acknowledge S. Sportelli, S. Briguglio, E. Giovannozzi, F. Zonca and C. Cosentino for encouragement and suggestions. This work has been carried out within the framework of the Nonlinear Energetic Particle Dynamics (NLED) European Enabling Research Project, WP 15-ER-01/ENEA-03, within the framework of the EUROfusion Consortium and has received funding from the Euratom research and training programme 2014-2018 under grant agreement No 633053. The views and opinions expressed herein do not necessarily reflect those of the European Commission.

Di Troia, C. (2018) Non-Perturbative Guiding Center and Stochastic Gyrocenter Transformations: Gyro-Phase Is the Kaluza-Klein 5^{th} Dimension also for Reconciling General Relativity with Quantum Mechanics. Journal of Modern Physics, 9, 701-752. https://doi.org/10.4236/jmp.2018.94048

From

Γ ˜ b c a = 1 2 g ˜ a e ( ∂ c g ˜ e b + ∂ b g ˜ c e − ∂ e g ˜ b c ) , (207)

with

g ˜ a b = | g α β − κ A α − κ A β κ 2 A α A α + 1 / φ 2 | , (208)

it is possible to compute all the components of the Christoffel symbol.

Γ ˜ β δ α = Γ β δ α + κ 2 φ 2 2 g α η ( A δ F β η + A β F δ η ) , (209)

Γ ˜ β δ 4 = − κ 2 A α Γ β δ α + κ 3 φ 2 2 A δ A α F α β + κ 3 φ 2 2 A β A α F α δ + κ 2 ( ∂ β A δ + ∂ δ A β ) ,

Γ ˜ β 4 α = κ φ 2 2 g α η F β η , (210)

and

Γ ˜ 44 α = Γ ˜ 44 4 = 0. (211)

Last,

Γ ˜ α 4 4 = κ 2 φ 2 2 A δ F δ α , (212)

and

Γ ˜ α 4 4 = Γ ˜ 44 4 = 0. (213)

From the components of Γ the component R ˜ 44 of the Ricci tensor in 5D can be computed:

R ˜ 44 = R ˜ 4 a 4 a = R ˜ 444 4 + R ˜ 4 β 4 β = R ˜ 4 β 4 β , (214)

with

R ˜ 4 β 4 β = κ 2 φ 4 4 F α β F α β − 1 2 ∇ α ∇ α φ 2 (215)

The other components are

R ˜ α 4 = R ˜ α a 4 a = R ˜ α 44 4 + R ˜ α β 4 β = R ˜ α β 4 β (216)

with

R ˜ α β 4 β = κ φ 2 2 g δ η ∇ η F α δ + κ A α R ˜ 4 β 4 β . (217)

Finally,

R ˜ α β = R ˜ α a β a = R ˜ α 4 β 4 + R ˜ α δ β δ = R ˜ α β 4 β , (218)

explicitly

R ˜ α β = R α β − κ 2 φ 2 2 g δ η F α δ F β η + κ 2 A α A β R ˜ 44 + κ A α ( R ˜ β 4 − κ A β R ˜ 44 ) + κ A β ( R ˜ α 4 − κ A α R ˜ 44 ) − 1 2 φ 2 ∇ α ∇ β φ 2 = R α β − κ 2 φ 2 2 g δ η F α δ F β η + κ 2 A α A β R ˜ 44 + κ 2 φ 2 2 g δ η A α ∇ η F β δ + κ 2 φ 2 2 g δ η A β ∇ η F α δ .

Thus, the scalar curvature in 5D is

R ˜ = R − κ 2 φ 2 4 F α β F α β − 1 φ 2 ∇ α ∇ α φ 2 (219)

It is convenient to settle the following Klein-Gordon equation with the Laplace-Beltrami operator:

( ∇ α ∇ α + Λ ) φ 2 = 0, (220)

being Λ prop. to the cosmological constant. However, let’s consider the simplest case with Λ = 0 . In such case,

R ˜ = R − κ 2 φ 2 4 F α β F α β . (221)