The Study on the Phase Structure of the Paul Trap System ()

Jaouad Kharbach^{1}, Mohamed Benkhali^{1}, Mohamed Benmalek^{1}, Ahmed Sali^{1}, Abdellah Rezzouk^{1}, Mohammed Ouazzani-Jamil^{2}

^{1}Laboratoire de Physique du Solide, Faculté des Sciences Dhar El Mahraz, Université Sidi Mohamed Ben Abdellah, Fès-Atlas, Morocco.

^{2}Université Privée de Fès, Laboratoire Systèmes et Environnements Durables, Lot. Quaraouiyine Route Ain Chkef, Fès, Morocco.

**DOI: **10.4236/am.2017.84042
PDF
HTML XML
1,126
Downloads
1,867
Views
Citations

In this article, the classic dynamic of Paul trap problem is investigated. We give a complete description of the topological structure of Hamiltonian flows on the real phase space. Using the surgery’s theory of Fomenko Liouville tori, all generic bifurcations of the common level sets of the first integrals were described theoretically. We give also an explicit periodic solution for singular values of the first integrals. Numerical investigations are carried out for all generic bifurcations and we observe order-chaos transition when the critical value of a control parameter is varied.

Keywords

Hamiltonian System, Integrability, Bifurcation, Liouville Tori, Periodic Solutions, Poincaré Section, Chaos

Share and Cite:

Kharbach, J. , Benkhali, M. , Benmalek, M. , Sali, A. , Rezzouk, A. and Ouazzani-Jamil, M. (2017) The Study on the Phase Structure of the Paul Trap System. *Applied Mathematics*, **8**, 525-536. doi: 10.4236/am.2017.84042.

1. Introduction

In recent years, the study of dynamic systems has been undertaken in a wide range of fields, which are located at the crossroads of differential geometry, algebraic geometry, number theory, Lie algebra, Intellectual and material means.

A considerable renewed interest appeared for Hamiltonian dynamic systems with two degrees of freedom, one of which is the study of the topological properties of the flow of these systems, their integrability, their chaotic behavior, the study of Periodic solutions and their bifurcation.

A first fundamental task in this field was the search for integrable systems which give rise to non chaotic behavior. For a Hamiltonian system with n degrees of freedom, the most general definition is that of Liouville. In addition to direct analytical methods, various criteria are developed to determine candidates for integrability, namely the Painlevé criterion, the Ziglin criterion and the Poincaré sections.

Integrability is clearly a central issue in understanding the origins and implications of the behaviour of the dynamical systems. Physically interesting integrable systems are rare, and consequently, it stirs up considerable excitement when one is discovered. Moreover, the Painlevé analysis as described in [1] [2] has been contributing -for some time now-a great deal in this direction.

Most integrable problems characterizing the motion of a rigid body around a fixed point were collected in [3] , furthermore, the study by Mikhail P. Kharlamov et al. and A.V. Tsiganov et al., as described in [4] [5] has been contributing for some time already in this direction and others types integrable problems describing the motion of a particle in the Euclidean plane were also collected in the Hietarinta study [6] nevertheless the problems correspond to the trapping of Ions [7] [8] , and new integrable problems in this field have been added by many authors.

We examine here an integrable mechanical system which exhibits a great richness of behavior. The proposed system is the system of Paul trap, the Hamiltonian flows are generated by the Hamiltonian:

$H\left(q,p,\lambda \right)=\frac{1}{2}\left({P}_{x}^{2}+{P}_{y}^{2}+{P}_{z}^{2}\right)+\frac{1}{r}+\frac{1}{2}\left({x}^{2}+{y}^{2}+{\lambda}^{2}{z}^{2}\right)$ (1)

where $\lambda $ is a constant, and $r=\sqrt{{x}^{2}+{y}^{2}+{z}^{2}}$ , is known to be integrable in the following three cases [9] : $\lambda =\pm 0.5,\pm 1,\pm 2$ it is also demonstrated that the ion dynamics in a Paul trap can be classified into four dynamical regimes [10] . This classification seems to be rather universal and shows up in the dynamics of periodically perturbed polar molecules, the hydrogen atom in strong magnetic fields [11] , and the periodically perturbed hydrogen atom.

The plan of the paper is as follows: In Section 2 we give a detailed description of the real phase space topology of the system (1) in the integrable $\lambda =\pm 1$ case, for doing that, we separate the Hamiltonian system from two canonical transformations. This separability implies a description of the topology of the common-level sets of the first integrals (invariant level sets) however, in our study we consider the common-level sets ${\mathcal{M}}_{\mathbb{R}}$ of the first integrals:

${\mathcal{M}}_{\mathbb{R}}=\left\{\left(x,y,z,{P}_{x},{P}_{y},{P}_{z}\right)\in {\mathbb{R}}^{6};H=h,F=f\right\}$ (2)

where H and F are respectively the Hamiltonian and the second invariant of the system.

According to the classical Liouville theorem, for noncritical values of the first integrals h and f, the regular level sets ${\mathcal{M}}_{\mathbb{R}}$ of a completely integrable Hamiltonian system consists of tori. All generic bifurcations of these tori, corresponding to these critical values will be described by using Fomenko theorem [12] . We also give in Section 2.3 an explicit periodic solution for singular level sets of bifurcation studied above. Finally, for nonintegrable regimes we carry out a numerical analysis to bring out the order-chaos transition.

In the Hamiltonian (1) there is a singularity at $r=0$ , which necessitates an infinitesimally small step size for numerical integration of the corresponding equation of motion. So, one has to introduce appropriate coordinate transformation to remove this singularity. For this purpose, you can use two canonical transformations, the first is:

$\{\begin{array}{l}x=\rho \mathrm{cos}\left(\phi \right),\text{\hspace{0.17em}}{P}_{x}={P}_{\rho}\mathrm{cos}\left(\phi \right)-{P}_{\phi}\frac{\mathrm{sin}\left(\phi \right)}{\rho}\\ y=\rho \mathrm{sin}\left(\phi \right),\text{\hspace{0.17em}}{P}_{y}={P}_{\rho}\mathrm{sin}\left(\phi \right)+{P}_{\phi}\frac{\mathrm{cos}\left(\phi \right)}{\rho}\\ z=z,\text{\hspace{0.17em}}{P}_{z}={P}_{z}\end{array}$ (3)

here ${P}_{\rho},{P}_{\phi}$ and ${P}_{z}$ are the canonical momenta conjugate to the coordinates $\rho ,\phi $ and $z$ respectively.

Then, Equation (1) Can be rewritten as for $\lambda =\pm 1$

$H=\frac{1}{2}\left({P}_{\rho}^{2}+{P}_{z}^{2}\right)+\frac{1}{2}\left({\rho}^{2}+{z}^{2}\right)+\frac{1}{r}+\frac{{P}_{\phi}^{2}}{2{\rho}^{2}},\text{\hspace{0.17em}}\text{\hspace{0.17em}}r=\sqrt{{\rho}^{2}+{z}^{2}}$ (4)

Equation (4) is a three degrees of freedom Hamiltonian system in which $\phi $ is a cyclic variable, and so the corresponding canonically conjugate momenta ${P}_{\phi}$ is conserved, or ${P}_{\phi}=m=\text{const}\text{.}$

Then, Equation (4) can be rewritten as

$H=\frac{1}{2}\left({P}_{\rho}^{2}+{P}_{z}^{2}\right)+\frac{1}{2}\left({\rho}^{2}+{z}^{2}\right)+\frac{1}{r}+\frac{{m}^{2}}{2{\rho}^{2}}$ (5)

the second canonical transformation is:

$\{\begin{array}{l}\rho =r\mathrm{cos}\left(\theta \right),\text{\hspace{0.17em}}{P}_{\rho}={P}_{r}\mathrm{cos}\left(\theta \right)-{P}_{\theta}\frac{\mathrm{sin}\left(\theta \right)}{r}\\ z=r\mathrm{sin}\left(\theta \right),\text{\hspace{0.17em}}{P}_{z}={P}_{r}\mathrm{sin}\left(\theta \right)+{P}_{\theta}\frac{\mathrm{cos}\left(\theta \right)}{r}\end{array}$ (6)

Then, Equation (5) can be rewritten as

$H=\frac{1}{2}{P}_{r}^{2}+\frac{1}{2{r}^{2}}{P}_{\theta}^{2}+\frac{1}{2}\frac{{m}^{2}}{{r}^{2}{\left(\mathrm{cos}\left(\theta \right)\right)}^{2}}+\frac{1}{2}{r}^{2}+\frac{1}{r}$ (7)

and the Hamilton’s equations of motion of (7) start as

$\{\begin{array}{l}\frac{\text{d}r}{\text{d}t}=\stackrel{\dot{}}{r}={P}_{r},\text{\hspace{0.17em}}\frac{\text{d}{P}_{r}}{\text{d}t}={\stackrel{\dot{}}{P}}_{r}=\frac{{P}_{\theta}^{2}}{{r}^{3}}-r+\frac{1}{{r}^{2}}\\ \frac{\text{d}\theta}{\text{d}t}=\stackrel{\dot{}}{\theta}=\frac{{P}_{\theta}}{{r}^{2}},\text{\hspace{0.17em}}\frac{\text{d}{P}_{\theta}}{\text{d}t}={\stackrel{\dot{}}{P}}_{\theta}=0\end{array}$ (8)

which is obtained by making ${P}_{\phi}=m=0$ .

2. Topological Analysis

In the integrable $\lambda =\pm 1$ case, we recall the Hamilton-Jacobi equation corresponding to the system (8) that separates into $r,\theta $ coordinates defined by

$\rho =r\mathrm{cos}\left(\theta \right),\text{\hspace{0.17em}}z=r\mathrm{sin}\left(\theta \right)\text{\hspace{0.17em}}\text{and}\text{\hspace{0.17em}}\phi =\text{const}$ (9)

It is easy to check that ${P}_{r}$ and ${P}_{\theta}$ can be expressed in terms of $r$ and $\theta $ characteristic polynomials in the following way:

$\{\begin{array}{l}{P}_{r}=\pm \frac{1}{r}\sqrt{G\left(r\right)}\\ {P}_{\theta}=\pm \sqrt{Q\left(\theta \right)}=\pm \sqrt{2F}=\text{const}\end{array}$ where #Math_34# (10)

And F denotes the second integral of motion:

$F={r}^{2}h-\frac{1}{2}{r}^{2}{P}_{r}^{2}-\frac{1}{2}{r}^{4}-r=\frac{1}{2}{P}_{\theta}^{2}$ (11)

$F=f=\frac{1}{2}{\left(\rho {P}_{z}-z{P}_{\rho}\right)}^{2}=\text{const}$ (12)

With the rescaled time variable: $\text{d}t=\frac{\text{d}\tau}{r}.$

Therefore, the differential equations satisfied by $r$ and $\theta $ are:

$\{\begin{array}{l}\frac{\text{d}r}{\sqrt{G\left(r\right)}}=\text{d}\tau \\ \frac{\text{d}\theta}{\sqrt{Q\left(\theta \right)}}=\text{d}t\end{array}$ (13)

2.1. Topology of Regular Level Set

In order to give a complete description of the topology of ${\mathcal{M}}_{\mathbb{R}}$ , we find first the bifurcation diagram B in the $\left(h,f\right)$ -plane, i.e. the set of the critical values of the energy-momentum mapping

$\left(\rho ,z,{P}_{\rho},{P}_{z}\right)\to \left(H,F\right)$ (14)

Definition. The bifurcation diagram of an integrable system is defined to be the region of possible motion depicted on the plane of first integrals $\left(h,f\right)$ [13] .

It turns out (like in the Hénon-Heils [14] , Gorjatchev-Tchaplygin top [15] , Fokker-Planck system [16] [17] and Kolossoff potential [18] [19] , the phase topology of a special case of Goryachev integrability in rigid body dynamics [20] ) that B is exactly the discriminant locus of the polynomial $G\left(r\right)$ whose coefficients are functions of h and f.

$B=\left\{\left(h,f\right)\in {\mathbb{R}}^{2}:\text{discriminant}\left(G\left(r\right)\right)=0\right\}$ (15)

where

$B=\left\{\left(h,f\right)\in {\mathbb{R}}^{2}:128{h}^{3}-432+512{h}^{4}f-2048{h}^{2}{f}^{2}-2304hf+2048{f}^{3}=0,f=\frac{1}{2}{P}_{\theta}^{2}\ge 0\right\}$

The set ${\mathcal{M}}_{\mathbb{R}}\backslash B$ consists of three connected components (as it is shown in Figure 1). Thus, in each connected component of the set ${\mathcal{M}}_{\mathbb{R}}\backslash B$ the level set ${\mathcal{M}}_{\mathbb{R}}$ has the same topological type and this latter may be changed only if $\left(h,f\right)$ passes through B.

Figure 1. Bifurcation diagram B.

As θ is acyclical variable $\Rightarrow \theta \in \left[0,2\text{\pi}\right].$

Theorem. The set ${\mathcal{M}}_{\mathbb{R}}\backslash B$ consists of three connected and nonintersecting with each other domains. The topological type of ${\mathcal{M}}_{\mathbb{R}}$ is a disjoint union of two-dimensional two-tori 2T, two-dimensional tori T and the empty set $\varphi $ .

Proof. Consider the complexified system

${\mathcal{M}}_{\not\subset}=\left\{\left(X,P\right)\in {\not\subset}^{4};H=h,F=f\right\}$ (16)

consider also the elliptic curves

${\Gamma}_{1}:\left\{{\omega}_{1}^{2}=G\left(r\right)\right\}$ and ${\Gamma}_{2}:\left\{{\omega}_{2}^{2}=Q\left(\theta \right)\right\}$ (17)

and the corresponding Riemann surfaces ${R}_{1}$ and ${R}_{2}$ of the same genus. We obtain the explicit solutions of the initial problem (13) by solving the Jacobi inversion problem [21] .

Define the natural projection

$\pi :{\mathcal{M}}_{\not\subset}\to {\Gamma}_{1}\otimes {\Gamma}_{2}$ (18)

(where Ä is the symmetric product), and the complex conjugation on ${\mathcal{M}}_{\not\subset}$

$\xi :\left(\rho ,z,{P}_{\rho},{P}_{z}\right)\to \left(\stackrel{\xaf}{\rho},\stackrel{\xaf}{z},{\stackrel{\xaf}{P}}_{\rho},{\stackrel{\xaf}{P}}_{z}\right)$ (19)

Consider also the natural projection $\eta $ on the Riemann surface $R={R}_{1}\otimes {R}_{2}$ given in $\left(r,\theta \right)$ coordinates by $\eta :\left(r,\theta \right)\to \left(\stackrel{\xaf}{r},\stackrel{\xaf}{\theta}\right)$ .

It induces an involution on the Jacobi variety and hence on ${\mathcal{M}}_{\not\subset}$ by the natural projection $\pi $ . By Equations (10) and (13) imply that this involution $\eta $ coincides with the complex conjugation (19) on ${\mathcal{M}}_{\not\subset}$ . The upshot is that in order to describe ${\mathcal{M}}_{\mathbb{R}}$ it is enough to study the projection:

$\pi :{\mathcal{M}}_{\not\subset}\to Jac\left(R\right)={\Gamma}_{1}\otimes {\Gamma}_{2}$ (20)

Definition. A connected component of the set of fixed points of $\tau $ on the curve ${\Gamma}_{1}$ and ${\Gamma}_{2}$ is called an oval.

To determine the ovals of ${\Gamma}_{1}$ and ${\Gamma}_{2}$ it suffices to study the real roots of the polynomial $G\left(r\right)$ for different values of h and f as shown in Table 1. Using the Formulae (10), and the condition that $\left(\rho ,z,{P}_{\rho},{P}_{z}\right)\in {\mathbb{R}}^{4}$ we find exactly two admissible ovals whose projections on the $r\u2013plan$ and $\theta -plan$ are given by ${\Delta}_{1}$ and ${\Delta}_{2}$ (see Table 2). The product of the admissible ovals in ${\Gamma}_{1}\otimes {\Gamma}_{2}$ and the projection $\pi $ of ${\mathcal{M}}_{\mathbb{R}}$ such as,#Math_89#, gives :

1) ${\mathcal{M}}_{\mathbb{R}}$ is a two-dimensional two-tori 2T in domain 3.

2) ${\mathcal{M}}_{\mathbb{R}}$ is a two-dimensional tori T in domain 2.

3) ${\mathcal{M}}_{\mathbb{R}}$ is the empty set in domain 1.

2.2. Topology of Singular Level Sets

Suppose now that the constants h and f are changed in such a way that $\left(h,f\right)$ passes through the bifurcation diagram B. Then the topological type of ${\mathcal{M}}_{\mathbb{R}}$ may change and the bifurcation of Liouville tori takes place. In order to describe all generic bifurcations of Liouville tori, we use Fomenko’s theorem of bifurcation for Liouville tori. We can have in our case two types of bifurcation (see Figure 2).

To prove that, it suffices to look at the bifurcations of roots of the polynomial $G\left(r\right)$ , the correspondence between bifurcation of roots and Liouville tori is shown in Figure 2.

Figure 2. Correspondence between bifurcations of roots of polynomial. $G\left(r\right)$ and bifurcations of invariant Liouville tori.

Table 1. Topological type of ${\mathcal{M}}_{\mathbb{R}}$ and the real roots of the polynomials $G\left(r\right)$ for $\left(h,f\right)\in {\mathbb{R}}^{2}\backslash B$ .

Table 2. Admissible ovals and topological type of ${\mathcal{M}}_{\mathbb{R}}$ for $\left(h,f\right)\in {\mathbb{R}}^{2}\backslash B$ .

2.3. Periodic Solutions

When the bifurcation of Liouville tori takes place, the level set ${\mathcal{M}}_{\mathbb{R}}$ becomes completely degenerate. Then we can have exceptional families of periodic solutions. It is seen from Table 3 that if $\left(h,f\right)$ is on the smooth curves ${C}_{0}$ (see Figure 1), ${\mathcal{M}}_{\mathbb{R}}$ contains a isolated circle S which is periodic solution. Consider now a fixed periodic solution belonging to the curve ${C}_{0}$ . The parameter $\theta $ takes values in the admissible interval $\left[0,2\text{\pi}\right]$ and r is equal to the double root of the polynomial $G\left(r\right)$ , ${r}_{1}={r}_{2}=k$ (see Table 3).

Then we obtain from (9) and (10) the following parameterization of fixed periodic solution:

$\{\begin{array}{l}\rho =k\mathrm{cos}\theta ,\text{\hspace{0.17em}}{P}_{\rho}=-\frac{\mathrm{sin}\theta}{k}\sqrt{Q\left(\theta \right)}\\ z=k\mathrm{sin}\theta ,\text{\hspace{0.17em}}{P}_{z}=\frac{\mathrm{cos}\theta}{k}{P}_{\theta}\end{array}$ (21)

Knowing that

$Q\left(\theta \right)={P}_{\theta}^{2}=2f$ (22)

The expression of ${P}_{\rho}$ can put in the form:

${P}_{\rho}=-\frac{\mathrm{sin}\left(\theta \right)}{k}\sqrt{2f}$ (23)

Using the differential equations of Hamilton

$\text{d}t=\frac{\text{d}\theta}{\sqrt{Q\left(\theta \right)}}=\frac{\text{d}\theta}{\sqrt{2f}}\Rightarrow \theta =\sqrt{2f}t$ (24)

It is easy to deduce solution

$z\left(t\right)=k\mathrm{sin}\left(\sqrt{2f}t\right)$ (25)

and the period associated is given by

${T}_{\theta}=\frac{2\text{\pi}}{\sqrt{2f}}$ (26)

3. Numerical Illustration

Using a surface of the section map, we give numerical illustrations of the topological analysis studied in Section 2.

For fixed values of energy h and f varies, the Liouville tori contained in the level set $H=h$ and $F=f$ change their topological type. The surfaces of section map shown in Figure 3 gives an illustration of the sequence of bifurcations

(a) (b) (c) (d) (e) (f) (g) (h) (i)

(j) (k) (l) (m) (n) (o) (p)

Figure 3. Surfaces of section map for different values of h, f and $\lambda $ , $\left({q}_{1},{p}_{1},{q}_{2},{p}_{2}\right)=\left(r,{P}_{r},\theta ,{P}_{\theta}\right)$ : (a) Domain 2 (h = 3.016, f = 3.345) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (b) Domain 2 (h = 3.016, f = 4.493) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (c) Domain 2 (h = 3.016, f = 3.345, 4.493, 5.023, 5.156, 5.377) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (d) Domain 2 (h = 3.016, f = 3.345, 4.493, 5.023, 5.156, 5.377) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (e) Domain 2 (h = 3.016,, f = 3.345, 4.493, 5.023, 5.156, 5.377) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (f) Domain 2 (h = 0.718, f = 0.828) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (g) Domain 2 (h = 0.718, f = 0.828) ${\mathcal{M}}_{\mathbb{R}}~T$ ; (h) Domain 2 (h = 1.997, f = 4.077) ${\mathcal{M}}_{\mathbb{R}}~S$ ; (i) Domain 2 (h = 1.997, f = 4.052) ${\mathcal{M}}_{\mathbb{R}}~S$ ; (j) View 2D of domain 2 (λ = 1.16); (k) View 3D of domain 2 (λ = 1.16); (l) Domain 2 (λ = 1.35); (m) Domain 3 (h = 4.041, f = 3.017) ${\mathcal{M}}_{\mathbb{R}}~2T$ ; (n) Domain 3 (h = 3.128, f = 3.017) ${\mathcal{M}}_{\mathbb{R}}~2T$ ; (o) Domain 3 (h = 3.0755, f = 3.017) ${\mathcal{M}}_{\mathbb{R}}~T\cup S$ ; (p) View 3D of domain 3 (λ = 1.18).

Table 3. Topological type of ${\mathcal{M}}_{\mathbb{R}}$ for $\left(h,f\right)\in B$ .

of Liouville tori and the order-chaos transition when one of the system parameters is varied. This map is constructed using a clever method introduced by Poincaré and extended by Hénon [22] .

The Figures 3(a)-(e) represent the sections for five values of the second invariant $f=3.345,4.493,5.023,5.156,5.377$ and $h=3.016$ . These values correspond to five points of domain 2 on the bifurcation diagram B where ${\mathcal{M}}_{\mathbb{R}}$ is a two-dimensional tori T. Moreover, the Figure 3(f) and Figure 3(g) show the sections for a value of the second invariant $f=0.828$ and $h=0.718$ . This value corresponds to a point in domain 2 on the bifurcation diagram B where ${\mathcal{M}}_{\mathbb{R}}$ is a two-dimensional T.

The fixed points in Figure 3(h) and Figure 3(i) show the sections representing the periodic solution where ${\mathcal{M}}_{\mathbb{R}}$ is an isolated circle S for $h=1.997$ and $f=4.077,4.052$ on the curve ${C}_{0}$ of B.

The Figure 3(m) show the sections for a value of the first invariant $h=4.041$ and $f=3.017$ . These values correspond to a point of Domain 3 on the bifurcation diagram B where ${\mathcal{M}}_{\mathbb{R}}$ is a two-dimensional two-tori 2T.

The Figure 3(n) and Figure 3(o) show the sections corresponding to the bifurcation on the curve ${C}_{1}$ of B for $h=3.0755,3.128$ and $f=3.017$ where ${\mathcal{M}}_{\mathbb{R}}$ is a $T\cup S$ .

For critical values of a control parameter $\lambda =1.16,1.35,1.18$ , we observe a fairly random distribution of points which correspond to a dramatic change in the Poincarésections indicating the order-chaos transition, as it is shown respectively on the Figure 3(j), Figure 3(k), Figure 3(l), and Figure 3(p).

4. Conclusions

In this study we have treated the classical dynamics of an integrable Hamiltonian system with two degrees of freedom. The system is characterized by a polynomial dependent on the invariants of the motion H and F. The different results obtained show the capacity of the method used to provide precise information on this Hamiltonian system. We have shown how this system can be converted by canonical transformations to easily exploitable Hamiltonians.

The very important question that we have studied is the topological analysis of the real invariant manifolds of the system. Fomenko’s theory on surgery and bifurcations of the Liouville tori has been combined with that of the algebraic structure to give a rigorous and detailed description of the topology of the invariant manifolds. For noncritical values of H and F, the variety contains torus or is empty.

In the same way we have shown how the periodic orbits can be found for singular values of first integrals, how the period of solutions is determined, and how explicit formulas can be established.

We have also highlighted numerically the topology of the invariant manifolds, the bifurcations of the Liouville tori and the order-chaos transition when the system control parameter varies.

Conflicts of Interest

The authors declare no conflicts of interest.

[1] |
Bountis, T.C. (1992) What Can Complex Time Tell Us about Real Time Dynamics. International Journal of Bifurcation and Chaos, 2, 217-228.
https://doi.org/10.1142/S0218127492000239 |

[2] |
Ramani, A., Grammaticos, B. and Bountis, T. (1989) The Painleve Property and Singularity Analysis of Integrable and Non-Integrable Systems. Physics Reports, 180, 159-245. https://doi.org/10.1016/0370-1573(89)90024-0 |

[3] | Borisov, A.V. and Mamaev, I.S. (2005) Rigid Body Dynamics. Hamiltonian Methods, Integrability, Chaos. Institute of computer Science, Moscow, 576. |

[4] |
Mikhail, P., Kharlamov, P.E., Ryabov, A. and Yu, S. (2016) Topological Atlas of the Kowalevski-Sokolov Top. Regular and Chaotic Dynamics, 21, 24-65.
https://doi.org/10.1134/S1560354716010032 |

[5] |
Tsiganov, A.V. (2010) On the Generalized Integrable Chaplygin System. Journal of Mathematical Sciences, 168, 901-911. https://doi.org/10.1007/ s10958-010-0036-5 |

[6] |
Hietarinta, J. (1987) Direct Methods for the Search of the Second Invariant. Physics Reports, 147, 87-154. https://doi.org/10.1016/0370-1573(87)90089-5 |

[7] |
Yaremko, Y., Przybylska, M. and Maciejewski, A.J. (2015) Dynamics of a Relativistic Charge in the Penning Trap. Chaos: An Interdisciplinary Journal of Nonlinear Science, 25, 053102-1-16. http://dx.doi.org/10.1063/1. 4919243 |

[8] |
Lanchares, V., Pascual, A.I., Palacián, J., Yanguas, P. and Salas, J.P. (2002) Perturbed Ion Traps: A Generalization of the Three-Dimensional Hénon-Heiles Problem. Chaos: An Interdisciplinary Journal of Nonlinear Science, 12, 87-99.
https://doi.org/10.1063/1.1449957 |

[9] | Baumann, G. and Nonnenmacher, T.F. (1992) Regular and Chaotic Motions in Ion Traps: A Nonlinear Analysis of Trap Equations. Physics Reports, A46, 2682-2692. |

[10] |
Blümel, R., Chen, J.M., Diedrich, F., Peik, E., Quint, W., Schleich, W., Shen, Y.R. and Walther, H. (1988) Phase Transitions of Stored Laser-Cooled Ions. Nature, 334, 309-313. https://doi.org/10.1038/334309a0 |

[11] | Wang, D. (2010) Dynamics of a Rydberg Hydrogen Atom in a Generalized van der Waals Potential and a Magnetic Field. Chinese Physics Letters, 27, 2. |

[12] |
Fomenko, A.T. (1988) Integrability and Nonintegrability in Geometric and Mechanics. Kluwer Academic Publisher, Heidelberg.
https://doi.org/10.1007/978-94-009-3069-8 |

[13] | Bolsinov, A.V., Borisov, A.V. and Mamaev, I.S. (2010) Topology and Stability of Integrable Systems. Russian Mathematical Surveys, 65, 259-317. |

[14] | Gavrilov, L. (1989) Bifurcations of the Invariant Manifolds in the Generalised Hénon-Heils System. Physical, D34, 223-239. |

[15] | Ouazzani, A.T.H., Kharbach, J., Dekkaki, S. and Ouazzani-Jamil, M. (2000) Bifurcations Sets of the Motion of a Heavy Rigid Body around a Fixed Point in Goryatchev-Tchaplygin Case. IL Nuovo Cimento, 115, 1175-1193. |

[16] |
Kharbach, J., Dekkaki, S., Ouazzani, A.T.H. and Ouazzani-Jamil, M. (2001) Topology and Bifurcations of the Invariant Level Sets of a Fokker-Planck Hamiltonian through Two Coupled Anisotropic Quartic Anharmonic Oscillators. Journal of Physics A: Mathematical and General, 34, 3437-3446.
https://doi.org/10.1088/0305-4470/34/16/312 |

[17] |
Kharbach, J., Dekkaki, S., Ouazzani, A.T.H. and Ouazzani-Jamil, M. (2003) Bifurcations of the Common Level Sets of Atomic Hydrogen in Van Der Waals Potential. International Journal of Bifurcation and Chaos, 13, 107-114.
https://doi.org/10.1142/S0218127403006364 |

[18] | Gavrilov, L., Ouazzani-Jamil, M. and Caboz, R. (1992) Bifurcations des Tores de Liouville du potentiel de Kolossoff . Comptes Rendus de l'Académie des Sciences, 315, 289-294. |

[19] |
Gavrilov, L., Ouazzani-Jamil, M. and Caboz, R. (1993) Bifurcation Diagrams and Fomenko's Surgery on Liouville Tori of the Kolossoff Potential . Annales scientifiques de l'école normale supérieure, 36, 545-564.
https://doi.org/10.24033/asens.1680 |

[20] | Ryabov, P.E. (2014) The Phase Topology of a Special Case of Goryachevintegrability in Rigid Body Dynamics. Sbornik: Mathematics, 205, 1024-1044. |

[21] |
Griffiths, P. and Harris, J. (1994) Principles of Algebraic Geometry. Wiley Interscience, New York. https://doi.org/10.1002/9781118032527 |

[22] |
Hénon, M. (1982) On the Numerical Computation of Poincaré Maps. Physical 5, 412-414. https://doi.org/10.1016/0167-2789(82)90034-3 |

Journals Menu

Contact us

+1 323-425-8868 | |

customer@scirp.org | |

+86 18163351462(WhatsApp) | |

1655362766 | |

Paper Publishing WeChat |

Copyright © 2023 by authors and Scientific Research Publishing Inc.

This work and the related PDF file are licensed under a Creative Commons Attribution 4.0 International License.