Research Article | Open Access
V. A. Malyshev, A. A. Zamyatin, "One-Dimensional Coulomb Multiparticle Systems", Advances in Mathematical Physics, vol. 2015, Article ID 857846, 9 pages, 2015. https://doi.org/10.1155/2015/857846
One-Dimensional Coulomb Multiparticle Systems
We consider the system of particles with equal charges and nearest neighbour Coulomb interaction on the interval. We study local properties of this system, in particular the distribution of distances between neighbouring charges. For zero temperature case there is sufficiently complete picture and we give a short review. For Gibbs distribution the situation is more difficult and we present two related results.
Many electric phenomena are not well understood and even might seem mysterious. More exactly, most are not still deduced from the microscale version of Maxwell equations on rigorous mathematical level. For example, even in the standard direct or alternative current, the electrons move along hundred kilometers of power lines, but the external accelerating force acts only on some meters of the wire. Here what one can read about this in “The Feynman Lectures on Physics” (see , volume 2, 16-2):
“…The force pushes the electrons along the wire. But why does this move the galvanometer, which is so far from the force? Because when the electrons which feel the magnetic force try to move, they push - by electric repulsion - the electrons a little farther down the wire; they, in turn, repel the electrons a little farther on, and so on for a long distance. An amazing thing. It was so amazing to Gauss and Weber - who first built a galvanometer - that they tried to see how far the forces in the wire would go. They strung the wire all the way across the city….”
This was written by the famous physicist Richard Feynman. However, after that, this “amazing thing” was vastly ignored in the literature. For example, the Drude model (that can be found in any textbook on solid state physics, see, e.g., ), considers free (noninteracting) electrons and constant external accelerating force acting along all the wire, without mentioning where this force (or field) comes from.
Many more questions arise. For example, why the electrons in DC move slowly, but such stationary regime is being established almost immediately. In [3, 4] it was demonstrated rigorously that even on the classical (not quantum) level that the stationary and space homogeneous flow of charged particles may exist as a result of self-organization of strongly interacting (via Coulomb repulsion) system of electrons. This means that the field accelerating the electrons is created by the neighboring electrons via some multiscale self-organization.
In fact, Ohm’s law is formulated on the macroscale (of order one); one-dimensional movement of electrons is described on the microscale (of order ), but the accelerating force is the corollary of the processes on the so-called submicroscale (of the order ). To show this we used not only classical nonrelativistic physics, Newtonian dynamics and Coulomb’s law, but also the simplest friction mechanism, ignoring where this friction mechanism comes from.
Besides other nonsolved dynamic problems like discharge, lightning, global current, bioelectricity, and so forth, also local and global properties of equilibrium configurations of charged particles in external electric fields are not at all studied (note that the mathematical part of equilibrium statistical physics has been developed mostly on the lattice). The equilibrium configurations can be either ground state (zero temperature) or Gibbs states. Ground states are easier to describe and we give short review of results in Section 2 of the paper. Study of local structure of Gibbs configurations is at the very beginning and we present in Section 3 two new results with complete proofs.
2. Part I: Ground State Configurations
Consider systems of particles with equal charges, Coulomb interaction and external force on an manifold. Even when there is no external force, the problem appears to be sufficiently difficult and was claimed important already long ago . For example, J. J. Thomson (who discovered electron) suggested the problem of finding such configurations on the sphere, and the answer has been known for = 2, 3, and 4 for more than 100 years, but for the solution was obtained only quite recently .
More interesting is the case of large , where the asymptotics is of main interest. In one-dimensional case T. J. Stieltjes studied the problem with logarithmic interaction and found its connection with zeros of orthogonal polynomials on the corresponding interval (see [7, 8]). However, the problem of finding minimal energy configurations on two-dimensional sphere for any and power interaction (sometimes it is called the seventh problem of Smale; it is also connected with the names of F. Risz and M. Fekete) was completely solved only for quadratic interaction (see [9–11] and review ). For more general compact manifolds see review .
In this section we review recent results concerning nonzero external force. Moreover, we consider not only global minima but even more interesting case of local energy minima. It appears that even in the simpler one-dimensional model with nearest neighbour interaction there is an interesting structure of fixed points (more exactly, fixed configurations), rich both in the number and in the charge distribution.
2.1. The Model
We consider the set of configurations of point particles:with equal charges on the segment . Here is assumed to be sufficiently large. We assume repulsive Coulomb interaction of nearest neighbours and external force ; that is, the potential energy is given bywhere , are positive constants. This defines the dynamics of the system of charges, if one defines exactly what occurs with particles and in the points and correspondingly. Namely, we assume completely inelastic boundary conditions. More exactly, when particle at time reaches point , having some velocity , then its velocity immediately becomes zero, and the particle itself stays at point until the force acting on it (which varies accordingly to the motion of other particles) becomes negative. The same occurs for the particle at point .
2.2. Problem of Many Local Minima
It is evident that if , then there is only one fixed point withThus it is the global energy minimum. More general result is the following.
Theorem 1. Assume that is continuous, nonnegative, and monotonic. Then for any , , and the fixed point exists and is unique.
However, the monotonicity assumption in this theorem is very essential. An example of strong nonuniqueness (where the number of fixed points is of the order ) is very simple—for a function with the only maximum inside the interval. Namely, on the interval , put for Then there exists such that for all sufficiently large and , one can show using similar techniques that for any odd there exists fixed point such thatMoreover, any such point will give local minimum of the energy.
One-dimensional case shows what can be expected in multidimensional case, which is more complicated but has great interest in connection to the static charge distribution in the atmosphere or in the living organism.
2.3. Phase Transitions
To discover phase transitions one should consider asymptotics , with the parameters being fixed. Then the fixed points will depend only on the “renormalized force” , and we assume that the renormalized constant can tend to infinity together with , namely, as , where .
The necessity to consider cases when depends on issues from concrete examples, where . For example, the linear density of electrons in some conductors, see , is of the order m−1, , and (volt/meter) where (in SI system). Thus has the order . This is close to the critical point of our model, which, as it will be shown, is asymptotically that is close to in our case.
Critical Force. For any there exists such that for the fixed point the following holds: for and for . If , then for any we have . At the same time , where
Multiscale Phase. The case when does not depend on was discussed in detail in [14, 15]; there are no phase transitions, but it is discovered that the structure of the fixed configuration differs from (3) only on the submicroscale of the order . More exactly, consider more general case when . Then the following holds: if does not depend on , then for any
Uniform Density. We define the density so that for any subintervals there exist the limitsThen if , then the density exists and is strictly uniform, that is, for all as ,
Nonuniform Density. If and , then and the density of particles exists and is nowhere zero but is not uniform (not constant in ).
Weak Contraction. If and , then, as ,and the density on the interval is not uniform.
Strong Contraction. If , then the density in the sense of distributions.
Both contraction cases are related to the discharge possibility; as after disappearance of the external force, discharge can be produced, the strength of which depends on the initial concentration of charged particles.
3. Part II: Gibbs Distribution
We consider the set , of configurations of points particles on the segment such thatIntroducing new variables , one sees that is an open simplex:which is denoted by .
We will consider the probability density:on with respect to the Lebesgue measure on , whereis the function on the set of configurations called the energy and is the function on the segment , called potential. The most interesting case for us is the Coulomb repulsive potential:Equivalently one could say that we consider the sumof independent identically distributed positive random variables , each having density , further assumed to be smooth, for simplicity. Then the conditional density of the vector , under the condition ,that coincides with (13), if we putIt is clear that conditional distributions are the same for all . In particularNote that in the limiting case the distribution is concentrated in the unique fixed point .
Below we put . Letbe the times convolution of . Then the conditional variance is
We want to note here that there exist many papers, related to the famous Kac mean field model, where conditional independence (chaos) of is proved under various conditions (see, e.g.,  and the references therein). We follow here another goal, that is, revealing possible multiscale local structure in the Gibbs situation, which could resemble zero temperature case structure, discussed in Section 2.
We consider the densities having the following asymptotic behaviour as :
Theorem 2. Under this condition and if and , as ,for some constant depending only on .
Theorem 3. If , then for any , as ,for some constant depending only on .
It is of interest to know the behaviour of the covariance for densities with hyperexponential decrease at zero.
3.2.1. General Power Asymptotics
We will prove here Theorem 2. Instead of one density it is useful to consider the family of densities (such trick has been used in some large deviations problems, see [18, 19])where andLet be random variables with density . Put , and denote the conditional densities of under the condition that :It is easy to check that in fact does not depend on .
Lemma 4. (1) and as . (2) there exists a unique , such that . Then , as .
Proof. (1) By abelian theorem, see [20, page 445, Theorem 3], and the condition as we have as It follows thatas .
(2) The function is monotonically decreasing in . Thus for any there exists such thatFrom (1) it follows that and as .
Let be the characteristic function of .
Lemma 5. The family of densities (25) has the following properties: (1)The normalized moment is bounded uniformly in .(2)For any there exists such that .(3)For some
Proof. (1) It is similar to the proof of (1) in Lemma 4.
(2) PutLet us show that for some as . For this we can write aswhereTaking into account thatand condition as we have that as Putting in the last integral we getAs for some , thenFor we get the estimateFrom these estimates (33) follows.
(3) Note that alwaysfor some . Without loss of generality one can assume that . By Hausdorff-Young inequalitywhere and . Asand , then
Lemma 6. Assume conditions (1)–(3) of Lemma 5 and that are defined by the condition . Thenwhere tends to uniformly in .
Proof. We change a bit the standard proof of local limit theorem. Let be the density of the standard deviationwhere is the sum independent random variables having density (25). Let be the standard Gaussian density. The inverse Fourier transform giveswhere . Denotewhere is bounded uniformly in (Lemma 5, part (1)). ThenFor we have the estimate (see [21, page 109, lemma 1])For we have by parts (2) and (3) of Lemma 5,for being sufficiently large, where and .
The estimate for is trivial. Thus,where does not depend on . Lemma follows asThe lemma is proved.
Lemma 7. Assume conditions (1)–(3) of Lemma 5. Then the conditional variancewhere
By Lemma 4 as . Thuswhere
Lemma 8. As ,
3.2.2. Coulomb Case
Again we introduce the exponential family of densitieswhere the function satisfies condition (22) with and
We will use modified Bessel function of the second kind defined as follows:where and . For we know the asymptotic expansion as :
Let again be a random variable with the density and put and .
Lemma 9. (1) As ,(2) As ,(3) There exists a unique such that such that and as .
Proof. (1) We can writewhereand is small enough. By (22)as . One can writewhereFind asymptotics of as . Changing variable givesand changing variable in (70) givesPut . Thenand using (71) we getTaking into account and for some small enough we come to (72).
(2) Mathematical expectation isBy part (1) of this lemma we haveSoCovariance is equal toIt follows from part (1) that, as ,Using asymptotic expansion (71) we getas .
(3) It follows from continuity of as function of and (85) that there exists such that and then as . By (88)Lemma is proved.
Lemma 10. The exponential family (68) has the following properties: (1)The normalized moment is bounded uniformly in .(2)For any there exists such that .(3)For some , as ,
Proof. It is similar to Lemma 5.
Using Lemmas 6, 7, and 9 we findwhereBy Lemma 9 and as , thenWe split the integral in (93) into two integrals: By condition (22)To find the asymptotics of we use Laplace’s method. Consider the function . Its derivativeequals at the point . The second derivativeThe function can be expanded at the neighborhood of using Taylor’s formula:By (72) we haveand so we get, as ,After cancellationsas . For the second integral we have, as ,SoTheorem is proved.
Conflict of Interests
The authors declare that there is no conflict of interests regarding the publication of this paper.
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