# Mean Field Approximation for the Dense Charged Drop.

1. IntroductionCollisions of relativistic nuclei in the RHIC and LHC experiments at very high energies led to the discovery of a new state of matter named quark-gluon plasma (QGP). At the initial stages of the scattering, this plasma resembles almost an ideal liquid whose microscopic structure is not yet well understood [1-11]. The data obtained in the RHIC experiments is in good agreement with the predictions of the ideal relativistic fluid dynamics [12-32], which establishes fluid dynamics as the main theoretical tool to describe collective flow in collisions. As an input to the hydrodynamical evolution of the particles, it is assumed that, after a very short time, [tau] < 1 fm/s [31, 32], the matter reaches a thermal equilibrium and expands with a very small shear viscosity [33-35].

In this paper, we continue to develop the model proposed in [36-39]. Namely, we assume that, at the local energy density fluctuations, hot drops [40-42] are created at the very initial stage of interactions at times [tau] < 0.5 fm. These fireballs (hot drops) are very dense and small, their size is much smaller than the proton size (see [36-39]), and their energy density is much larger than the density achieved in high-energy interactions at the energies [square root of (s)] < 100 GeV. In our model, we assume that the fireballs consist of particles with weak interparticle interactions and have a nonzero charge. We consider this drop of charged particles from the point of view of quantum statistical physics. The most general Hamiltonian for this system can be written in the form which describes all possible interactions between the particles in the drop:

H = [H.sup.0] + [V.sup.1] + [V.sup.2] + ... + [V.sup.i] + ... (1)

(see [43]), where as usual [V.sup.1] is the energy of interaction of the particle with an external field, [V.sup.2] is the energy of pair-like interactions, and so forth. The mean field approximation for the probe particle in the system of charged particles, therefore, can be introduced by the following perturbative scheme. First of all, we can consider the motion of only one probe particle in the mean field of all other particles, which corresponds to preserving only the [V.sup.1] term in the expression of (1). This approximation will lead to the modification of the propagator of the particle, namely, from a free propagator to some "dressed" one. At the next step, we can take two probe particles, each of which will propagate in the mean field of the other charges of the system, similar to the first approximation, but additionally we can introduce the interaction of these two particles one with another in the mean field of the remaining charges in the drop, which requires introduction of one [V.sup.2] term in the expression of (1) in the mean field approximation. Further, we can increase the number of the probe particles in the system, considering, in addition to pair interactions, the interactions of free probe particles and so on.

In the present calculations, we limit ourselves to the first order of the mean field approach; namely, we will consider the motion of one nonrelativistic probe particle in the external mean field created by all other particles in the charged drop.

2. Mean Field Approximation for the Hamiltonian of the System

In the absence of the external field, we write the Hamiltonian of the system of charged particles as

[mathematical expression not reproducible]. (2)

Here,

N = [integral] [[PSI].sup.+.sub.[alpha]](t, [??]) [[PSI].sub.[alpha]](t, [??]) [d.sup.3]x (3)

is a particle number operator. Considering the mean field approximation for a spherically symmetrical system, we introduce

[mathematical expression not reproducible] (4)

as some particles density for the droplet with characteristic size [r.sub.0]; here, r = [absolute value of [??]]. The f(r, r', [r.sub.0]) function is a distribution function of the system of interest; it can be correctly determined by writing the corresponding Vlasov or Boltzmann equations coupled to system (1). In our case, we will not consider a particular form of this function, but instead we will discuss its form based on some physical assumptions only. Therefore, we obtain the following for the Hamiltonian:

[mathematical expression not reproducible], (5)

which represents now the energy of the probe particle in the mean field created by the other particles of the system. Due to the spherical symmetry of the problem, we expand all the operators in the Hamiltonian expression in terms of spherical harmonic functions. We have the following for the two-particle interaction potential:

[mathematical expression not reproducible] (6)

with [PSI], [PHI] as spherical angles of r' vector, [psi], [phi] as spherical angles of r vector in some spherical coordinate system, and [theta](r) as the step function. Correspondingly, we write the particle-field operator as

[[PSI].sub.[alpha]](t, [??]) = [[infinity].summation over (l=0)][l.summation over (m=-l)] [[psi].sub.[alpha]lm](t, r) [Y.sub.lm]([psi], [phi]). (7)

Using the orthogonality property of the harmonic functions

[integral] [Y.sub.lm]([psi], [phi]) [Y.sup.*.sub.l'm']([psi], [phi])d[OMEGA] = [[delta].sub.ll'][[delta].sub.mm'], (8)

with [d.sup.3]x = [r.sup.2]dr d[OMEGA], we rewrite the Hamiltonian equation (5) in a one-dimensional form as a function of r and r' only:

[mathematical expression not reproducible]. (9)

In the next section, we solve Schrodinger's equation corresponding to this Hamiltonian.

3. Equations of Motion

We introduce the usual commutation relations for the fields of interest (see (7)):

[mathematical expression not reproducible]. (10)

Using the property of (8), we correspondingly obtain one-dimensional commutation relations for the new fields:

{[[psi].sub.[alpha]lm](t, r), [[psi].sup.+.sub.[beta]l'm](t, r')} = [1/[r.sup.2]] [[delta].sub.[alpha][beta]][[delta].sub.ll'][[delta].sub.mm'], [delta](r - r'). (11)

The Schrodinger equation for [[psi].sub.[alpha]lm](t, r) field, therefore, has the following form:

[mathematical expression not reproducible]. (12)

Rescaling the drop's density function and rewriting it in the dimensionless form as

f(r - r' - [r.sub.0]) [right arrow] [1/[r.sup.3/2][(r').sup.3/2]] f(r, r', [r.sub.0]), (13)

introducing a new variable in integrals in (12),

r' = xr, (14)

we rewrite the integrals in (12) finally as

[mathematical expression not reproducible]. (15)

For the case of the drop of small size, we can expand our [psi] function in (15) around x = 1 in both terms; this point gives the main contribution to both integrals. Therefore, in the first approximation, we have the following for (15):

[mathematical expression not reproducible], (16)

with [Q.sub.l] as an l multipole moment of the drop. The Schroodinger equation (12) now acquires the following form:

l [[partial derivative]/[partial derivative]t] [[psi].sub.[alpha]lm](t, r) = (-1/2m([[DELTA].sub.r] - l(l + 1)/[r.sup.2]) - [mu] + [[q.sup.2]/r] [Q.sub.l](r)) x [[psi].sub.[alpha]lm](t, r). (17)

Representing the wave function as

[[psi].sub.[alpha]lm](t, r) = [u.sub.[alpha]lm](r) [e.sup.-lt(E-[mu)], (18)

we obtain the Schroodinger equation for the particle in the following form:

([1/2m] [[DELTA].sub.r] - [1/2m] [l(l + 1)/[r.sup.2]] + E - [[q.sup.2]/r] [Q.sub.l](r)) [u.sub.[alpha]lm](r) = 0. (19)

In general, we cannot solve this equation without knowledge of the form of f(r, x, [r.sub.0]) particles distribution function in integrals of (15). Nevertheless, we can guess the form of the function in the r [less than or equal to] [r.sub.0] region of the drop, mostly interesting for us. Indeed, at r [much greater than] [r.sub.0], which is outside the drop region, the potential equation (16) is the usual Coulomb potential, but in the r [less than or equal to] [r.sub.0] region, the situation is different. The existence of the drop requires the presence of some potential well at r [less than or equal to] [r.sub.0] which will keep particles inside the drop for some (very short) time and, therefore, it must be the potential's minimum present somewhere between r = 0 and r [varies] [r.sub.0]. Hence, this minimum is the indication of the creation of the dense drop of finite size in the interaction system of interest and, consequently, we can write the potential energy from (19) in this region as

[mathematical expression not reproducible], (20)

where we assumed that the potential energy acquires its minimum at [r.sub.min]; [A.sub.l]([r.sub.min]) here are the positive coefficients of the potential's expansion around this minimum. This situation, in fact, is similar to the situation in the system of two-atom molecules (see [44] and the references therein), where two atoms are kept inside some mutual potential well. Inserting the expansion of (20) in (19), we obtain the following equation:

([1/2m] [[DELTA].sub.r] + E - [1/2m] [l(l + 1)/[r.sup.2.sub.min]] - [Q.sub.l]([r.sub.min]) [q.sup.2]/[r.sub.min] - [A.sub.l]([r.sub.min]) [q.sup.2]/2[r.sup.3.sub.0][(r - [r.sub.min]).sup.2])[u.sub.[alpha]lm](r) = 0. (21)

The solution of this equation is similar to the solution of the Schroodinger equation for the harmonic oscillator with energy levels defined by

E' = E - [1/2m] [l(l + 1)/[r.sup.2.sub.min]] - [Q.sub.l]([r.sub.min]) [q.sup.2]/[r.sub.min], (22)

and consequently the energy levels of the system are given by

[E.sub.nl] = [1/2m] [l(l + 1)/[r.sup.2.sub.min]] + [Q.sub.l]([r.sub.min]) [q.sup.2]/[r.sub.min] + q[([A.sub.l]([r.sub.min])/m[r.sup.3.sub.0]).sup.1/2](n + 1/2) n = 0, 1, 2, ..., (23)

with the wave functions

[mathematical expression not reproducible], (24)

where

R = [([r.sup.3.sub.0]/m[A.sub.l]([r.sub.min])[q.sup.2]).sup.1/4]. (25)

We note that the obtained solution is indeed similar to the solution of the Schrodinger equation for the two-atom molecules (see, e.g., [44]).

4. Conclusion

In this note, we demonstrated that the spectrum of the charged nonrelativistic particle in the dense charged drop has a quantum structure (see (23)), and it is determined by three terms in the first mean field approximation. The first term in (23) can be considered as the quantized rotation energy of the drop; the second one is the quantized electrostatic energy due to the multipole moments of the charged drop. The third term in the expression of (23) is the usual quantum corrections to the energy due to the oscillation of the particle inside the drop with eigenfrequencies determined by the form of the distribution function of the particles in the drop. The presence of this minimum is a necessary condition of the drop's creation (see also [36-39]). The values of these corrections have an additional degeneracy of energy levels defined by l quantum number in comparison to the ordinary quantum oscillator. In this formulation, the considered problem is similar to the problem of the description of the system of the two-atom molecule (see [44]) (we note that the proposed approach can be used also for the description of bound states created at low energy interactions, and we plan to investigate this subject in a separate publication). Further development of the approach can include the consideration of higher orders of mean field approximation for the system and introduction of the kinetic equation for the distribution function of (4) coupled to the Hamiltonian; we plan to consider these problems in the following publications.

We conclude that our model can be useful for the clarification of the spectrum of the produced particles, which is influenced by the quantum-mechanical properties of the QCD fireball. We believe that this approach will provide the connection between the data, obtained in high-energy collisions of protons and nuclei in the LHC and RHIC experiments [12-32, 45-49], and microscopic fields inside the collision region.

https://doi.org/10.1155/2017/7374909

Conflicts of Interest

The authors declare that there are no conflicts of interest regarding the publication of this paper.

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S. Bondarenko and K. Komoshvili

Ariel University, Ariel, Israel

Correspondence should be addressed to S. Bondarenko; sergeyb@ariel.ac.il

Received 22 October 2017; Revised 29 November 2017; Accepted 6 December 2017; Published 31 December 2017

Academic Editor: Edward Sarkisyan-Grinbaum

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Title Annotation: | Research Article |
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Author: | Bondarenko, S.; Komoshvili, K. |

Publication: | Advances in High Energy Physics |

Article Type: | Report |

Geographic Code: | 1USA |

Date: | Jan 1, 2018 |

Words: | 3498 |

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