_{1}

We present a class of non-convective classical solutions for the multidimensional incompressible Navier-Stokes equation. We validate such class as a representative for solutions of the equation in bounded and unbounded domains by investigating the compatibility condition on the boundary, the smoothness of the solution inside the domain and the boundedness of the energy. Eventually, we show that this solution is indeed the unique classical solution for the problem given some appropriate and convenient assumptions on the data.

In this article, a well known model is to be investigated that represents the flow of an incompressible fluid in both bounded and unbounded domains of ℝ N . This model is commonly called the Navier-Stokes equation following the French engineer Navier who was the first to propose this model. This model was investigated later by Poisson and de Saint Venant. However, Stokes was the one who justified the model based on the principles of continuum mechanics. By advent of 1930, the interest in this model increased significantly and outstanding results were obtained by Leray, Hopf, Ladyzhenskaya and Finn.

This equation describes the flow of what is so called the Newtonian fluid. These are the fluids that exhibit shearing stress due to the presence of frictional forces. Frictional forces within fluids are consequences of its viscosity. Also, the gradient of the velocity represents a measure for the relative motion of the fluid’s particles. Moreover, deformation of fluids is commonly associated with internal and external body forces; the internal force is what we refer to as the pressure of the fluid. The derivation of the Navier-Stokes equation is a natural application of Newton’s second law of motion, the balance of momentum and the mass conservation, which eventually leads to the definition of the Cauchy stress tensor. In Newtonian fluids, this stress tensor is a function in the pressure, the viscosity and the gradient of the velocity. For a convenient physical background about the basics of continuum mechanics and how we derive the Navier-Stokes equation we propose [

This model poses a serious challenge when it comes to proving the existence and the smoothness of its solution. This problem was perfectly addressed by Ladyzhenskaya in two dimensional spaces among many other issues in higher dimensional spaces [

Recently, the interest in this equation is not fading at all. There are persistent efforts to clarify the properties of the solution, especially its smoothness. Among many respectful results, we mention the outstanding analysis by Tao in [

In this article the idea is simple. A class of possible solutions is proposed and then it is proved that it indeed represents the unique classical solution of the problem. Most of the results are obtained by considering standard theories of partial differential equations. Some of the results in the monograph [

The spatial domain is Ω which is either a bounded region in ℝ N or the whole of ℝ N and this point shall be specified explicitly. For the sake of conciseness, the notation Ω t is used to denote Ω t = { ( x , t ) : x ∈ Ω , t ∈ ( 0 , ∞ ) } . Clearly, such notation should not be taken to imply a moving boundary. The main model equation is in the form

{ v t + ( v ⋅ ∇ ) v = μ Δ v − ∇ p + f in Ω t , ω = ∇ × v in Ω t , v ( x , 0 ) = v 0 ( x ) and ω 0 ( x ) = ∇ × v 0 ( x ) in Ω , v ( x , t ) = v * ( x N − 1 , t ) on ∂ Ω t , ∇ ⋅ v = ∇ ⋅ ω = 0 in Ω ¯ t (1)

where the last equation in the above model is what many authors commonly refer to as the incompressibility condition or the solenoidal condition. The first term in the first equation is the acceleration of the fluid’s flow in time, the second is the convective term that represents the acceleration of the flow in space, the third represents the diffusion scaled by the kinematic viscosity constant μ , the fourth is the pressure, and the last one represents the total of the external body forces. The initial profile is denoted by v 0 and the boundary datum is denoted by v * . The solution v is the vector field representing the velocity of the flow in each direction, and its rotation ω is the vorticity. Note that ∇ ⋅ ω = 0 in Ω ¯ t by compatibility.

The well known Lebesgue spaces L q ( Ω ) will be used repeatedly to represent the functions with bounded mean of order q. The Sobolev space H m ( Ω ) is used to represent functions with bounded derivatives such that for a vector field v = { v 1 , ⋯ , v N } one has ∂ | α | v i ∈ L 2 ( Ω ) for every | α | = 1 , ⋯ , m and i = 1 , ⋯ , N . This motivates the usage of the space V m ( Ω ) , which is a well known space of functions in the theory of incompressible fluids as a representative for divergence free (solenoidal) bounded vector fields such that V m ( Ω ) = { v ∈ H m ( Ω ) : ∇ ⋅ v = 0 in Ω } .

By laws of classical mechanics, the energy generated by a moving object is proportional to the square of its velocity. Hence, the energy E ( t ) generated by the flow v is defined as follows

E ( t ) = ∫ Ω | v ( x , t ) | 2 d x . (2)

Recall that the above integral represents the norm of v in the Lebesgue space L 2 ( Ω ) . The smoothness of v 0 ( x ) is such that

v 0 ( x ) ∈ C 2 ( Ω ¯ ) ∩ V N + 2 ( Ω ) . (3)

The smoothness of the boundary datum v * ( x N − 1 , t ) is such that

v * ( x N − 1 , t ) ∈ C ∞ ( ∂ Ω t ) and v * ( ⋅ , t ) ~ t − K * for any K * > 1. (4)

Finally, the forcing term f is smooth in space and time such that

f ( x , t ) ∈ C 1 ( [ 0, ∞ ] ; C 1 ( Ω ¯ ) ∩ H 3 ( Ω ) ) and f ( ⋅ , t ) ~ t − K for any K > 0. (5)

Note that the intersections in the above conditions are not really required in the case of bounded domain since boundedness of the domain and continuity of the functions are enough to imply boundedness in the sense of the mean. However, these requirements are of significant importance in the case of unbounded domain as will be shown later.

The target is to define a class of possible solutions to Model Equation (1) from which v , ω and p can be concluded. Once v is obtained, then p can easily be recovered from the main model. The validity of this solution as a meaningful physical solution will be investigated when inserted in the main model. A meaningful solution is a unique and smooth solution that vanishes as t → ∞ , and in the case of unbounded domain it vanishes as | x | → ∞ as well.

Remark. The curl operator or the rotation of a vector field has a physical meaning only in three dimensional space. However, it will be used in ℝ N for the sake of generality. Most of the results depend on the curl operator in the sense of a differential operator without direct exposure to its definition. Note that the main interest is to find the velocity, which means that any use of the rotation, in spite of its significance in this work, is nothing more than a transient step. It can always be assumed that the space is three dimensional when needed, and a generalization becomes possible by reverting back to the results of the velocity. In particular, some of the vorticity ideas introduced in [

In this section a class of possible solutions is proposed and the insertion of these solutions in the main model is investigated to check where they will lead to. This is initiated by the statement of the following claim.

Claim 1. The unique solution of Model Equation (1) is in the form v ( x , t ) = ψ ( x , t ) u ( t ) where ψ : ℝ N × ℝ → ℝ is a scalar field and u = ( u 1 ( t ) , ⋯ , u N ( t ) ) is a vector field such that, at least, ψ ( x , t ) ∈ C 2 ( Ω ¯ t ) and u ∈ C ( ℝ ) .

An important question in the theory of Navier-Stokes equation is the ability to verify the compatibility condition on the boundary with minimum restrictions on the flux passing through the boundary especially if ∂ Ω is divided into several parts ( [

∫ ∂ Ω ( v ⋅ n → ) d x N − 1 = 0, (6)

where n → is the outward unit vector normal to ∂ Ω . This motivates the introduction of the following lemma.

Lemma 1 (Tangential flow). Let Ω be an arbitrary domain, ψ ( x , t ) : ℝ N × ℝ → ℝ be any scalar field such that ψ ∈ C 1 ( Ω ¯ ) and let u ( t ) = ( u 1 ( t ) , ⋯ , u N ( t ) ) be any vector field independent of x . The Compatibility Condition (6) is satisfied for every divergence free vector field v ( x , t ) : ℝ N × ℝ → ℝ N in the form v = ψ ( x , t ) u ( t ) . In particular, on every part of ∂ Ω , v and its rotation ω are tangents to ∂ Ω such that v ⋅ n → = ω ⋅ n → = 0 .

Proof. Given that v = ψ ( x , t ) u ( t ) is divergence free such that ∇ ⋅ v = 0 leads to

∑ i = 1 N ∂ ψ ∂ x i u i = 0. (7)

Identity (7) can be used to deduce that ( v ⋅ ∇ ) v = ( ∇ v ) v = 0 . Upon dot product by v one obtains

0 = ( ∇ v ) v ⋅ v = ( ∇ v ) T v ⋅ v = 1 2 v ⋅ ∇ | v | 2 = 1 2 ∇ ⋅ ( | v | 2 v ) , (8)

and when integrated over Ω for any t > 0 provides

0 = ∫ Ω ∇ ⋅ ( | v | 2 v ) d x = ∫ ∂ Ω ( | v | 2 v ⋅ n → ) d x N − 1 , (9)

which is a true identity for every arbitrary Ω , ψ and u and for every t > 0 . On the other hand, given that ( v ⋅ ∇ ) v = 0 , one can use the identity

1 2 ∇ | v | 2 = ( v ⋅ ∇ ) v + v × ∇ × v = v × ω , (10)

where ω = ∇ × v , which upon dot product by ω provides

∇ ⋅ ( | v | 2 ω ) = 0,

where we used also that ∇ ⋅ ω = 0 . Integrate over Ω for any t > 0 to get

0 = ∫ Ω ∇ ⋅ ( | v | 2 ω ) d x = ∫ ∂ Ω ( | v | 2 ω ⋅ n → ) d x N − 1 , (11)

which is true for arbitrary Ω , ψ and u . Now, since ∇ ⋅ v = 0 one also has

0 = ∫ Ω ( ∇ ⋅ v ) d x = ∫ ∂ Ω ( v ⋅ n → ) d x N − 1 . (12)

Identity (10) implies that ∇ | v | 2 is orthogonal to the space spanned by v and ω . Combine Identities (9), (11) and (12), and exclude the cases | v | = 1 and | v | = 0 by the arbitrariness of the choice to deduce that it is necessary that v ⋅ n → = 0 ; that is to say v is tangential to every part of ∂ Ω . It can also be deduced that either v = ω on every part of ∂ Ω (this actually means v = ω = 0 on ∂ Ω ), or ω ⋅ n → = 0 on every part of ∂ Ω . Both cases imply that ω ⋅ n → = 0 on every part of ∂ Ω . Hence, both v and ω are tangential to the boundary.

Remark. As pointed out, the question of verifying the Compatibility Condition (6) on the boundary of Ω is an important open question in the mathematical theory of Navier-Stokes equation. Some results were obtained to justify the validity of such compatibility under certain restrictions on the flux of the flow in terms of the viscosity of the fluid, for details on this issue refer to [

Theorem 2 (Bounded Domain). Let Ω ⊂ ℝ N be a bounded domain with sufficiently smooth boundaries ∂ Ω and let Ω t = Ω × ( 0 , ∞ ) . Suppose v 0 ( x ) , v * ( x N − 1 , t ) and f ( x , t ) satisfy Conditions (3), (4) and (5) respectively. If v ( x , t ) is in the form proposed in Claim 1, then Model Equation (1) has a classical solution ( v , ω , p ) with bounded energy E ( t ) such that v ( x , t ) ∈ C ∞ ( Ω ¯ t ) , ω ( x , t ) ∈ C ∞ ( Ω ¯ t ) and p ( x , t ) ∈ C 1 ( [ 0, ∞ ] ; C 3 ( Ω ¯ ) ) . In particular, the exact solution is given by solving the following system

{ ω t = μ Δ ω + ∇ × f Δ v = − ∇ × ω Δ p = ∇ ⋅ f } in Ω t , v ( x , t ) = v * ( x N − 1 , t ) ω ( x , t ) = ∇ × v * ( x N − 1 , t ) } on ∂ Ω t , ω ( x , 0 ) = ω 0 ( x ) = ∇ × v 0 ( x ) in Ω ¯ , ∇ ⋅ v = ∇ ⋅ ω = 0 in Ω ¯ t (13)

where ∇ p can be defined uniquely in terms of the values of v and f on the boundary. Moreover, if f ∈ C ∞ ( Ω ¯ t ) then p ∈ C ∞ ( Ω ¯ t ) .

Proof. The proof is quite simple and it depends mostly on classical results and the standard theory of linear parabolic and elliptic equations of second order. If v = ψ ( x , t ) u ( t ) , then by virtue of Identity (7) one has ( v ⋅ ∇ ) v = 0 . Hence, the main equation takes the form

v t = μ Δ v − ∇ p + f . (14)

Apply the divergence operator to get

Δ p = ∇ ⋅ f , (15)

where the incompressibility condition ∇ ⋅ v = 0 is used. By the standard theory of elliptic equations, if f satisfies Condition (5), then p ∈ C 1 ( [ 0, ∞ ] ; C 3 ( Ω ¯ ) ) . However, if f ∈ C ∞ ( Ω ¯ t ) , then p is actually C ∞ ( Ω ¯ t ) , for details on such equation see ( [

Now, revert to Equation (14) and apply the curl operator to get

ω t = μ Δ ω + ∇ × f , (16)

which is the first equation in System (13). Finally, given the incompressibility of v and applying a simple vector identity lead to the third equation in System (13) that is

− Δ v = ∇ × ω . (17)

The fundamental solution ω to Equation (16) with initial profile ω 0 and force ∇ × f is given formally by

ω ( x , t ) = ( 4 π μ t ) − N 2 ∫ Ω e − | x − y | 2 4 μ t ∇ × v 0 ( y ) d y + ∫ 0 t ( 4 π μ ( t − s ) ) − N 2 ∫ Ω e − | x − y | 2 4 μ ( t − s ) ∇ × f ( y , s ) d y d s . (18)

As explained in ( [

Now, go back to Equation (17). By virtue of the results obtained above for ω and the standard theory of elliptic equations one directly concludes that v ∈ C ∞ ( Ω ¯ t ) , for more details see ( [

v ( x , t ) = 1 ω N ∫ Ω x − y | x − y | N × ω ( y , t ) d y , (19)

where ω N is the area of the unit sphere in ℝ N . The solution v can be enforced to take the values v * on the boundary in a standard manner by introducing Dirichlet Green’s function. We refrain from discussing these details being highly dependent on the choice of the domain. The uniqueness of v follows by the presence of the boundary condition v * , for details see [

Finally, go back to Equation (15) to solve for p . In this case one only needs to calculate ∇ p ⋅ n → from the main model by knowing the values of v t , Δ v and f on the boundary. This provides a form of boundary conditions for p which consequently guarantees its uniqueness up to a constant, for details see [

Remark. As explained in the proof of Theorem 2, the uniqueness of ω follows by the ability to define v uniquely. The order of solving the equations in System (13) is not really important since none of the quantities ( v , ω , p ) induces the other; they act simultaneously. Another way of solvability can be introduced by which one can obtain the same results. This can be a topic for a future study.

The problem of proving the existence of regular and smooth enough solutions for the Navier-Stokes equation in bounded domain was exhaustively investigated as pointed out in the introduction. The real problem was to prove the boundedness of the solution in an unbounded domain, clearly because of the unboundedness of the domain itself. This fact manifests the need to show that the solution’s support is bounded in ℝ N , or equivalently to show that the solution v decays rapidly as | x | → ∞ .

The solution obtained in Theorem 2 represents a perfect candidate as a solution for Model Equation (1) in unbounded domains also except for one issue. One needs to prove the boundedness of v in L 2 ( ℝ N ) for every t > 0 so that the boundedness of the energy E ( t ) can be claimed, and also to ensure that the solution does indeed vanish as | x | → ∞ . For v to be bounded in L 2 ( ℝ N ) , it should attain a rate of decay, at least, | v | ≤ C ( 1 + | x | ) − ( N + δ ) / 2 for any δ > 0 . One can argue that some of the results in the literature require a rate of decay higher than that for the surface integrals to vanish; these restrictions can be dropped because these integrals already vanish by virtue of Lemma 1, (see [

In order to derive such an estimate one goes back to Formula (19) that represents the fundamental solution for v . If | ω | ≤ C then it is expected that the outcome of this integral will provide nothing less than a linear rate of growth for | v | , which is a bad answer to the problem in hand. Therefore, Formula (18) shall be used to help us estimate some rates of decay for ω and consequently for v so that boundedness in L 2 ( Ω ) can be proved for every t > 0.

Theorem 3 (The Domain R^{N}). Suppose all the conditions of Theorem 2 are satisfied for Ω = ℝ N . Then there exists a classical solution ( v , ω , p ) for Model Equation (1) represented by the System (13) and defined as

ω ( x , t ) = h ( t ) ∫ ℝ N e − | x − y | 2 4 μ t ω 0 ( y ) d y + ∫ 0 t h ( t − s ) ∫ ℝ N e − | x − y | 2 4 μ ( t − s ) g ( y , s ) d y d s , (20)

and

v ( x , t ) = 1 ω N ∫ ℝ N x − y | x − y | N × ω ( y , t ) d y , (21)

where h ( t ) = ( 4 π μ t ) − N 2 , g = ∇ × f and ω N is the surface area of a unit

sphere. The pressure p can be defined from Model Equation (1) up to a constant where ∇ p ⋅ n → can be specified uniquely in terms of the values of v and f on the boundary. Moreover, the energy of the flow E ( t ) is bounded for every t > 0 where v grows at most as | v | ~ ( 1 + | x | ) − ( N + 6 ) / 2 .

Proof. The proof of smoothness and uniqueness is identical to the one introduced in the proof of Theorem 2 and it follows by the standard theory of linear second order elliptic and parabolic equations. The focus here will be on proving the boundedness in L 2 ( ℝ N ) for both ω and v , which necessarily entails an estimation of appropriate decay rates as pointed out in the preceding discussion. Since f ∈ C 1 ( [ 0, ∞ ] ; H 3 ( ℝ N ) ) , then g ∈ C ( [ 0, ∞ ] ; H 2 ( ℝ N ) ) . By assumption, v 0 ∈ V N + 2 ( ℝ N ) which implies that ω 0 ∈ V N + 1 ( ℝ N ) and since N ≥ 2 for meaningful physical interpretation, then at least ω 0 ∈ V 3 ( ℝ N ) . Hence, ω ∈ L 2 ( ( 0, ∞ ] ; V 4 ( ℝ N ) ) as per the standard theory of linear second order parabolic equations, for details refer to ( [

The first direction depends on the results in ( [

∫ 0 T | ω ( x , t ) | L ∞ ( Ω t ) d t ≤ C

and such that v ∈ C 1 ( ( 0, T ] ; C 2 ( Ω ) ∩ V m ( Ω ) ) . Since ω 0 and g are bounded in L 2 ( ℝ N ) for every t > 0 , then it follows that there exists a ball B ⊂ ℝ N such that the supports of g and ω 0 are entirely inside B t where B t = B × [ 0 , ∞ ] . Hence, the integrals in Formula (20) can be restricted to the ball B , apply Hölder’s inequality, maximize the exponential term which is bounded for every x , y ∈ B and for every t > 0 , and with some estimation procedures it becomes easy to find an estimate of the form | ω ( x , t ) | ≤ C h ( t ) in the whole of ℝ N and for every t > 0 . Since h ( t ) is a decreasing function in time then by assuming a simple scale of time one obtains

∫ 0 ∞ | ω ( x , t ) | L ∞ ( Ω ¯ t ) d t ≤ C ∫ 1 ∞ h ( τ ) d τ ≤ C .

It follows that all the conditions of ( [

The second way is trying to get an estimate for v in terms of | x | to confirm the boundedness in L 2 ( ℝ N ) . Consider the following argument: fix t in Expression (20), calculate ∇ ω , which is in L 2 ( ℝ N ) for every t > 0 because ω ∈ V 4 ( Ω ) . Take the absolute value of both sides, perform some manipulation to the integrands, use x ⋅ y ≤ | x | | y | and maximize the time integral (the integrand is a decreasing function in time) so that one finally gets the term with the highest power for | x | as follows

| ∇ ω | ≤ H ( t ) ∫ B | x | ( | 1 + | y | | x | | 2 ) 1 2 e − | x − y | 2 4 μ t ( | ω 0 ( y ) | L ∞ ( B ) + | g ( y , t ) | L ∞ ( B t ) ) d y ≤ H ( t ) M ( | x | ) | x | C ( | B | , | ω 0 | L ∞ ( B ) + | g | L ∞ ( B t ) ) ≤ C M ( | x | ) | x | ,

where M ( | x | ) is the collection of every possible appearance of any power of | x | after the integration. Since ∇ ω is in L 2 ( ℝ N ) as pointed out, then to obtain a decreasing integrand when calculating the L 2 -norm of this derivative it is necessary that M ( | x | ) is decreasing in | x | such that it is at least

M ( | x | ) ~ ( 1 + | x | ) − N + 2 + δ 2 for some δ > 0 . But ω is in L 2 ( ℝ N ) as well, and the integrands of the above estimate are the same except for the terms with positive powers of | x | . That is to say that | ω | ≤ C M ( | x | ) ~ ( 1 + | x | ) − N + 2 + δ 2 . Incorporate this estimate in Expression (21) of the solution v and one can readily see that | v | ~ ( 1 + | x | ) − N + δ 2 as desired, which in turn confirms the boundedness of the energy E ( t ) for every t > 0 and implies the decay of v as | x | → ∞ .

However, since ω ∈ V 4 ( ℝ N ) , then we actually have D 4 ω ∈ L 2 ( ℝ N ) for every t > 0 . This means that we can differentiate Formula (20) four times and repeat the same argument as above to conclude that we actually have

M ( | x | ) ~ ( 1 + | x | ) − N + 8 + δ 2 which in turn leads to | v | ~ ( 1 + | x | ) − N + 6 + δ 2 and this

completes the proof.

Remark. Better estimates for the decay of v can be obtained by repeating the same procedure described above for higher order derivatives of ω which, of course, entails higher assumptions on the data so that we can claim the boundedness of the considered derivative apriori. On the other hand, the assumptions on the smoothness of the forcing term f can be relaxed. It is enough to assume that f ∈ C 1 ( [ 0, ∞ ] ; C 1 ( ℝ N ) ∩ H 1 ( ℝ N ) ) so that one obtains g ∈ C ( [ 0, ∞ ] ; L 2 ( ℝ N ) ) , which is sufficient to conclude that ω ∈ L 2 ( ( 0, ∞ ] ; V 2 ( ℝ N ) ) . The boundedness of ∇ ω in L 2 ( ℝ N ) is enough to deduce a sufficient decay estimate for v as shown above. The introduced assumptions were chosen for consistency with the standard theory and the Embedding Theorem, and in the same time to illustrate the estimation procedure. For more information review ( [

We managed to prove that our solution is indeed a classical solution of Model Equation (1). Here come some important questions, what if there exists another solution in a more general form? Moreover, does the choice of the domain or the choice of the boundary data play a role in the uniqueness of the solution? The answer to these questions is addressed by the statement of the next theorem.

Theorem 4 (Uniqueness). Let Ω ⊆ ℝ N be an arbitrary domain. Suppose v 0 , v * and f are satisfying Conditions (3), (4) and (5) respectively. Then Claim 1 is true and the unique classical solution of Model Equation (1) is in the form v ( x , t ) = ψ ( x , t ) u ( t ) . This solution is defined as per Theorems 2 and 3.

Proof. The proof here depends on our results in Theorems 2 and 3, and also on ( [

Assume that there exists a more general solution than the proposed one and denote it by v g . Such solution should definitely inherit the smoothness proved in [

w t − μ Δ w + ∇ q = ( v g ⋅ ∇ ) v g . (22)

Dot product the above equation by v g and integrate by parts over any arbitrary domain Ω to get

∫ Ω v g ⋅ ( w t − μ Δ w + ∇ q ) d x = 1 2 ∫ ∂ Ω | v g | 2 v g ⋅ n → d x N − 1 = 1 2 ∫ ∂ Ω | v | 2 v ⋅ n → d x N − 1 = 0 , (23)

where we used the Divergence theorem in the right hand side, the facts that ∇ ⋅ v g = 0 and that v g = v * = v on the boundary, and the results of Lemma 1. Now, recalling that ∇ ⋅ ω g = 0 and using the vector identity

∇ | v g | 2 = 2 ( v g ⋅ ∇ ) v g + 2 v g × ω g , (24)

one can dot product Equation (22) by ω g and integrate as above to get

∫ Ω ω g ⋅ ( w t − μ Δ w + ∇ q ) d x = 1 2 ∫ ∂ Ω | v g | 2 ω g ⋅ n → d x N − 1 = 1 2 ∫ ∂ Ω | v ∗ | 2 ∇ × v ∗ ⋅ n → d x N − 1 = 1 2 ∫ ∂ Ω | v | 2 ω ⋅ n → d x N − 1 = 0 , (25)

where Lemma 1 is used again. Identities (23) and (25) imply one of three possibilities. Either v g = ω g = 0 which is excluded for being trivial, or w t − μ Δ w + ∇ q = 0 almost everywhere. The third possibility is w t − μ Δ w + ∇ q being orthogonal to the space spanned by v g and ω g , which by Equation (22) implies that ( v g ⋅ ∇ ) v g is orthogonal to ω g and v g .

Let us start with w t − μ Δ w + ∇ q = 0 almost everywhere. Multiply this equation by w , integrate by parts over Ω , employ the Divergence theorem and recall that w = 0 on ∂ Ω to get

1 2 d d t ∫ Ω | w | 2 d x + μ ∫ Ω | ∇ w | 2 d x = − ∫ ∂ Ω q w ⋅ n → d x N − 1 = 0.

This readily implies that w = 0 almost everywhere. But by the results obtained for v and v g , one concludes that at least w ∈ C 2 ( Ω ¯ ) which implies that w is identically zero. Hence, the solution v is the unique solution for Model Equation (1) in this case.

Now, if v g and ω g are orthogonal to ( v g ⋅ ∇ ) v g , then by Identity (24) we deduce that ∇ | v g | 2 is orthogonal to the space spanned by v g and ω g everywhere, which is equivalent to the nature of the solution v . This means that ∇ | v | 2 and ∇ | v g | 2 are parallel to each other on the boundary. Since both solutions coincide at the boundary and both are extended continuously to the interior of the domain, then it is not hard to conclude that v g = v everywhere, which is the aim of this proof. Assume not. Let θ = ω − ω g so that the difference equation for ω takes the form

θ t − μ Δ θ = ( v g ⋅ ∇ ) ω g − ( ω g ⋅ ∇ ) v g . (26)

where ( ω g ⋅ ∇ ) v g − ( v g ⋅ ∇ ) ω g = − ∇ × ( v g ⋅ ∇ ) v g . Use the vector identity

∇ ( v g ⋅ ω g ) = ( ∇ v g ) T ω g + ( ∇ ω g ) T v g ,

and given the incompressibility of v g one also has

∇ ω g ω g = 1 2 ∇ | ω g | 2 − ω g × ( ∇ × ω g ) = 1 2 ∇ | ω g | 2 + ω g × Δ v g .

Use these two identities, bearing in mind the incompressibility, to find that

v g ⋅ ( ∇ ω g v g − ∇ v g ω g ) = ( ∇ ω ) T v g ⋅ v g − 1 2 ∇ | v g | 2 ⋅ ω g = ∇ ( v g ⋅ ω g ) ⋅ v g − ( ∇ v g ) T ω g ⋅ v g − 1 2 ∇ | v g | 2 ⋅ ω g = ∇ ⋅ ( ( v g ⋅ ω g ) v g − 1 2 | v g | 2 ω g ) − ∇ v g v g ⋅ ω g = ∇ ⋅ ( ( v g ⋅ ω g ) v g − 1 2 | v g | 2 ω g ) − 1 2 ∇ | v g | 2 ⋅ ω g + ( v g × ω g ) ⋅ ω g = ∇ ⋅ ( ( v g ⋅ ω g ) v g − | v g | 2 ω g ) = ∇ ⋅ G 1 ( v g , ω g ) . (27)

Now recall that we are discussing the possibility in which ∇ | v g | 2 is orthogonal to v g and ω g such that C ∇ | v g | 2 = ( v g × ω g ) . Following the same steps as above one can write

ω g ⋅ ( ∇ ω g v g − ∇ v g ω g ) = ∇ ⋅ ( | ω g | 2 v g − ( v g ⋅ ω g ) ω g ) − ( ω g × Δ v g ) ⋅ v g = ∇ ⋅ ( | ω g | 2 v g − ( v g ⋅ ω g ) ω g ) − ( v g × ω g ) ⋅ Δ v g = ∇ ⋅ ( | ω g | 2 v g − ( v g ⋅ ω g ) ω g ) − C ∇ | v g | 2 ⋅ Δ v g = ∇ ⋅ ( | ω g | 2 v g − ( v g ⋅ ω g ) ω g − C | v g | 2 Δ v g ) = ∇ ⋅ G 2 ( v g , ω g ) . (28)

Now, dot product Equation (26) by v g , use Identity (27), integrate over Ω and use the Divergence theorem to reach

∫ Ω v g ⋅ ( θ t − μ Δ θ ) d x = ∫ ∂ Ω G 1 ( v g , ω g ) ⋅ n → d x N − 1 = ∫ ∂ Ω G 1 ( v , ω ) ⋅ n → d x N − 1 . (29)

Also dot product Equation (26) by ω g , use Identity (28), integrate over Ω and use the Divergence theorem to get

∫ Ω ω g ⋅ ( θ t − μ Δ θ ) d x = ∫ ∂ Ω G 2 ( v g , ω g ) ⋅ n → d x N − 1 = ∫ ∂ Ω G 2 ( v , ω ) ⋅ n → d x N − 1 . (30)

Now, reverse the Divergence theorem in the surface integrals that include values of v and ω and reverse all the steps made to conclude G 1 and G 2 to obtain identities in the form

∫ Ω v g ⋅ ( θ t − μ Δ θ ) d x = ∫ Ω v ⋅ ∇ × ( ( v ⋅ ∇ ) v ) d x = 0, (31)

and similarly

∫ Ω ω g ⋅ ( θ t − μ Δ θ ) d x = ∫ Ω ω ⋅ ∇ × ( ( v ⋅ ∇ ) v ) d x = 0. (32)

Now, there are three other possibilities. The trivial solution; that is v g = ω g = 0 and it is excluded. Another one is θ t − μ Δ θ = 0 and this one is equivalent to w t − μ Δ w + ∇ q = 0 because the uniqueness of v implies the uniqueness of ω and vice versa. It remains that ∇ × ( ( v g ⋅ ∇ ) v g ) is orthogonal to the space spanned by v g and ω g . But we already have ( v g ⋅ ∇ ) v g orthogonal to v g and ω g , which implies that ( v g ⋅ ∇ ) v g and its rotation (curl) are parallel to each other. By definition, the curl operator is the unique vector field for which ( ∇ s − ∇ s T ) a = ( ∇ × s ) × a for every vector field a ( [

Remark. In the proof of uniqueness one can argue that the statement of the proof was given in the sense of classical solutions, and such that there still exists another solution in a weaker form. While this may sound true, but in fact it is not. The basic idea of the proof is based on using the coincidence on the boundary and then moving back to the interior. Assuming the existence of a weaker solution does not change the fact that it is going to coincide with the proposed one on the boundary. However, further investigation on this specific point will be introduced in a future study.

A class of possible solutions for the incompressible Navier-Stokes equation in bounded and unbounded regions of ℝ N is proposed. It was demonstrated that for such class of vector fields, the flux of the energy of the flow is orthogonal to the space spanned by v and its associated rotation ω . It was also proved that v and ω are tangential to the boundary such that v ⋅ n → = ω ⋅ n → = 0 .

An investigation of the validity of this class of vector fields as a candidate for a solution to the incompressible Navier-Stokes equation was carried out in both bounded and unbounded domains. Given plausible assumptions on the data and a forcing term in the case of unbounded domains, it turned out that this class of solutions represents perfectly a classical solution of the problem. Verification was established for the infinite differentiability, the uniqueness and the boundedness of the energy in appropriate spaces in light of well known and standard theories. An appropriate estimate was also given for the minimum rate of decay of the solution v as | x | → ∞ . Moreover, global existence in time and the corresponding rate of decay were quite obvious in the deduced formulas.

Finally, it was proved that this class of solutions represents actually the unique classical solution of the incompressible Navier-Stokes equation. In light of the non-convective nature of the proposed solution and the uniqueness argument under arbitrary settings, the incompressible Navier-Stokes equation can safely be reduced to a linear equation. This point is quite interesting and it motivates further investigations on a possible relation between incompressibility and convection in fluid mechanics.

Sincere thanks to the members of JAMP for their professional performance, and special thanks to managing editor Hellen Xu for a rare attitude of high quality.

Khedr, W.S. (2017) Classical Fundamental Unique Solution for the Incompressible Navier-Stokes Equation in R^{N}. Journal of Applied Mathe- matics and Physics, 5, 939-952. https://doi.org/10.4236/jamp.2017.54083