FiniteSize Effects in NonNeutral TwoDimensional Coulomb Fluids
Abstract
Thermodynamic potential of a neutral twodimensional (2D) Coulomb fluid, confined to a large domain with a smooth boundary, exhibits at any (inverse) temperature a logarithmic finitesize correction term whose universal prefactor depends only on the Euler number of the domain and the conformal anomaly number . A minimal free boson conformal field theory, which is equivalent to the 2D symmetric twocomponent plasma of elementary charges at coupling constant , was studied in the past. It was shown that creating a nonneutrality by spreading out a charge at infinity modifies the anomaly number to . Here, we study the effect of nonneutrality on the finitesize expansion of the free energy for another Coulomb fluid, namely the 2D onecomponent plasma (jellium) composed of identical pointlike charges in a homogeneous background surface charge density. For the disk geometry of the confining domain we find that the nonneutrality induces the same change of the anomaly number in the finitesize expansion. We derive this result first at the freefermion coupling and then, by using a mapping of the 2D onecomponent plasma onto an anticommuting field theory formulated on a chain, for an arbitrary coupling constant.
Keywords:
Coulomb fluidFinitesize correctionCentral chargeConformal field theory∎
1 Introduction
According to the principle of conformal invariance Affleck86 ; Blote86 ; Cardy88a , twodimensional (2D) systems of constituents with shortrange interactions, confined to a large domain with a smooth boundary, exhibit at the critical point universal finitesize properties. In particular, for a disk domain of radius , with the Euler number , the (dimensionless) free energy has the large expansion
(1.1) 
where is the inverse temperature and is a length scale. The bulk specific free energy and the surface tension are nonuniversal, i.e., dependent on microscopic details of the given model and on the temperature. The logarithmic term is universal, depending only on the conformal anomaly number (central charge) of the critical theory. Like for instance, the massless Gaussian theory with a field , defined by the Hamiltonian
(1.2) 
has Cardy88b .
In this paper, we study 2D classical (i.e., nonquantum) systems of charged pointlike particles interacting pairwisely by the longrange Coulomb potential , where the dielectric constants of the medium in which particles move and of the walls are equal to (vacuum in Gauss units), for simplicity. The logarithmic potential is the solution of the 2D Poisson equation
(1.3) 
and in three dimensions corresponds to the effective interaction of infinitely long parallel charged lines, perpendicular to the plane. Two types of Coulomb systems are of special interest. The onecomponent plasma (OCP), or jellium, is a system of identical mobile (say elementary) charges immersed in a homogeneous neutralizing background charge density. The symmetric twocomponent plasma (TCP), or the Coulomb gas, is a system of oppositely charged mobile particles with no background. While the OCP is usually studied in the canonical ensemble, the TCP is treated within the grandcanonical ensemble, with the enforced neutrality condition for each microscopic configuration. In both cases, the thermodynamics and the particle correlation functions are determined by the only dimensionless parameter, the coupling constant . The 2D OCP is exactly solvable at by mapping onto free fermions Jancovici81 . The 2D TCP undergoes the collapse of positivenegative pairs of pointlike charges at coupling , which corresponds to the exactly solvable freefermion point of the equivalent Thirring model Cornu87 ; Gaudin85 . For reviews about exactly solvable 2D Coulomb systems with various geometries of confining domains, see Refs. Forrester98 ; Jancovici92 .
At arbitrary temperature of the conducting regime, the longrange tail of the Coulomb potential induces screening. Due to the screening effect, the bulk particle correlations exhibit shortrange (exponential or even Gaussian) decay which indicates a noncriticality. On the other hand, the same screening phenomenon causes that the induced electricalfield correlations are longranged Jancovici95 ; Lebowitz84 . As a result, the free energy (or the grand potential) of any Coulomb system exhibits a universal finitesize correction of type (1.1). Since the logarithmic Coulomb potential is the inverse of the Laplacian operator , in the functional sense it is associated with the Gaussian Hamiltonian (1.2) rewritten as . Although the conformal anomaly number of Coulomb systems is expected to be related to the Gaussian one, there is a change of sign, namely
(1.4) 
The explicit checks of the universal finitesize behavior with were done, for both OCP and TCP, at the exactly solvable coupling . The studied cases involve Coulomb gases with periodic boundary conditions Forrester91 , confined to a domain by plain hard walls Jancovici94 , by idealconductor boundaries Jancovici96 and by idealdielectric walls Jancovici01 ; Tellez01 . For Coulomb systems living on a surface of the sphere, a direct derivation of the universal finitesize correction was performed for any coupling by combining stereographic projection of the sphere onto an infinite plane with linear response theory (TCP, Ref. Jancovici00a ) or with density functional approach (OCP, Ref. Jancovici00c ). The prefactor to the universal correction term was related to the second moment of the shortrange part of the planar direct correlation function. Using a renormalized Mayer expansion Deutsch74 ; Friedman62 and observing a cancellation property of specific families of renormalized diagrams, this second moment was evaluated for both TCP Jancovici00b and OCP Kalinay00 . Another explicit derivation of the universal logarithmic term at an arbitrary coupling constant was made for the TCP in a disk geometry Samaj02 . All obtained results confirm the conformal prediction (1.1) for a critical system as we had .
All that has been said holds for neutral Coulomb systems. Recently, Ferrero and Téllez Ferrero14 studied the 2D TCP of charges at the exactly solvable collapse point, confined to a disk of radius . They fixed a “guest” hardcore impurity of charge at the disk origin and found that the large expansion for the grand potential of type (1.1) applies if the conformal anomaly number is modified to
(1.5) 
presence of the impurity has no effect on bulk and boundary terms. It has been noted in the same reference that the same modification of the anomaly number occurs when the minimal free boson conformal field theory Dotsenko04 ; Ginsparg89 , equivalent formally to the 2D TCP, is deformed by spreading out a charge at infinity, creating in this way a nonneutral system. The equivalence of the two systems, one with a charge fixed at the disk origin and one with the same charge spread out at infinity, can be explained by noting that a charge fixed at the disk origin is screened at microscopic distances by counterions from the TCP and thus the universal large correction looks like the one for a nonneutral system with the net charge . Notice that the definition of in Refs. Dotsenko04 ; Ferrero14 has opposite sign with respect to the standard notation used in this paper. At an arbitrary , conformal field theory Dotsenko04 ; Ginsparg89 yields
(1.6) 
With this conformal number, the logarithmic correction in (1.1) is no longer universal, its prefactor depends on both the coupling constant and the excess charge.
In this paper, we concentrate on the nonneutral 2D OCP confined to the disk. We perform a microscopic derivation of the finitesize expansion of the free energy and find that it is of type (1.1) with the same anomaly number (1.6) as found for the 2D TCP in the context of conformal field theories. We would like to note that in contrast to the previous studies Jancovici03 ; Levesque00 ; Martin80 of charge fluctuations in finite Coulomb systems in a much larger overall neutral system or with particle reservoir put at infinity, here we consider nonneutral systems within the constrained canonical ensemble with the fixed net charge and look for the dependence of finitesize corrections of the free energy on this excess charge.
The paper is organized as follows. In Sect. 2, we derive the total energy of mobile charged particles and the fixed background in presence of nonneutrality. Section 3 summarizas the general mapping of the 2D OCP onto the theory of anticommuting variables on a onedimensional chain. The exactly solvable freefermion case is the subject of Sect. 4. The freefermion result is generalized to an arbitrary coupling in Sect. 5. In Sect. 6, we give a short recapitulation and some concluding remarks.
2 Derivation of Boltzmann factor
Let us consider the 2D OCP inside the disk of radius . There are pointlike particles of charge immersed in a uniform background charge density , where the background density is given by
(2.1) 
The net charge of the system is thus and the neutral case corresponds to . The particle density is given by
(2.2) 
As
(2.3) 
the particle and background densities coincide in the thermodynamic limit .
The potential induced by the background charge density reads as
(2.4) 
This potential satisfies the Poisson equation with circular symmetry
(2.5) 
The potential at the disk boundary is given by the total background charge placed at the origin, i.e., . The solution of Eq. (2.5), supplemented by this boundary condition, reads
(2.6) 
To derive the total Boltzmann factor, we proceed in close analogy with neutral systems, see e.g. Refs. DiFrancesco94 ; Forrester98 ; Sari76 . The total Coulomb interaction energy of the particlebackground system consists of three parts:

the particleparticle interaction
(2.7) 
the particlebackground interaction
(2.8) 
the backgroundbackground interaction
(2.9)
With the definition of the coupling constant , the corresponding Boltzmann factor reads as
(2.10)  
From the expression for the canonical partition function
(2.11) 
the free energy is given by , i.e.,
(2.12)  
Here,
(2.13) 
is the configuration integral with the circularly symmetric onebody Boltzmann factor
(2.14) 
3 Mapping onto 1D fermions
There exist two basic approaches how to treat the configuration integral (2.13). The first one is based on the expansion of the power of van der monde determinants in the basis of Jack polynomials Salazar16 ; Tellez99 ; Tellez12 . The second one is based on the mapping onto a 1D lattice fermion system; this formalism has been introduced in Ref. Samaj95 and developed further in Refs. Samaj00 ; Samaj04 ; Samaj11 ; Samaj14 ; Samaj15 ; Samaj16 . The relation between the two methods was established in Ref. Grimaldo15 . Here, we apply the mapping onto 1D fermions.
For a positive integer, the configuration integral (2.13) can be expressed in terms of two sets of anticommuting variables each with components , defined on a discrete chain of sites , as follows
(3.1) 
Here, and the action involves pair interactions of composite operators
(3.2) 
i.e. the products of anticommuting variables from a given set with the fixed sum of site indices. The elements of the diagonal interaction matrix are given by
(3.3) 
For the present onebody Boltzmann factor (2.14), the interaction strengths can be rewritten as follows
(3.4) 
The onebody density of particles at point is defined by
(3.5) 
where is the microscopic density of particles at point and denotes the statistical average over canonical ensemble. The onebody density can be obtained from the configuration integral (2.13) in the standard way as the functional derivative:
(3.6) 
Within the formalism of anticommuting variables, the circularly symmetric onebody density is expressible explicitly as
(3.7) 
where
(3.8) 
denotes averaging over anticommuting variables.
4 The freefermion point
For , the composite operators (3.2) are the ordinary anticommuting variables. The diagonalized action in (3.1) then implies
(4.1) 
Since the correlators
(4.2) 
the particle density (3.7) takes the form
(4.3) 
According to (3.4), the interaction strengths are expressible as
(4.4) 
Since
(4.5) 
the expression (2.12) for the free energy can be rewritten as
(4.6)  
Now we aim at estimating the crucial sum . Since it holds
(4.7) 
we get the important relation
(4.8) 
Consequently,
(4.9)  
where is the particle number density at , i.e., at the wall contact. We can write
(4.10) 
This formula completes the determination of the free energy (4.6).
Let us now consider the large limit when the background density is related to the particle density via . We start with the sum representation (4.10). With the aid of formulas presented in Appendix A of Ref. DiFrancesco94 , we find that
(4.11) 
Using the asymptotic formula Erdelyi
(4.12) 
with
(4.13) 
being the error function, we obtain Jancovici94
(4.14) 
Finally, the integral
(4.15) 
depends on the statistical average which is finite for any , and therefore in the limit contributes to . It is natural to suppose that in the limit the statistical averages do not depend on the finite charge imbalance within an infinite domain and so the particle density at the disk border tends to its halfspace “wall contact” value Jancovici82 , independent of . Thus we have
(4.16) 
which is the term of order . To summarize,
(4.17)  
Inserting this large formula into (4.6) and taking into account that
(4.18) 
we arrive at the finitesize expansion of type (1.1) with
(4.19) 
We see that for the coupling the central charge depends on in the same way as for the 2D TCP at the same coupling constant , see Eq. (1.5).
5 Arbitrary with integer
For an arbitrary integer , there exist certain analogies with the exactly solvable case.
In the configuration integral (3.1), we perform the unitary transformation of anticommuting variables, say ’s,
(5.1) 
which keeps the composite form of operators. Here, and are free asyet unspecified parameters. Taking into account the corresponding Jacobian, this transformation modifies to the form
(5.2) 
where
(5.3) 
Choosing
(5.4) 
we eliminate the dependent prefactor in (3.4) and in this way pass from to . We obtain that
(5.5) 
where
(5.6) 
To obtain a convenient representation of , we differentiate this quantity with respect to :
(5.7) 
Since
(5.8) 
we get
(5.9) 
As concerns the correlators , we return back to the original anticommuting ’s variables by applying the inverse to the transformation (5.1). The Jacobians of the numerator and the denominator cancel with one another and we obtain
(5.10) 
Consequently, the relation (5.7) takes the form
(5.11)  
As the result
(5.12) 
Putting together Eqs. (2.12), (5.5) and (5.12), the free energy is given by
(5.13)  
As before, the mean particle density at the disk border is finite for any and in the large limit we have
(5.14) 
In contrast to the case, the explicit value of is not known, but the important information is that this term is of order . Consequently,
(5.15) 
Considering for the neutral the anticipated critical finitesize expansion (1.1) with , the conformal anomaly number is equal to the one predicted by conformal field theory in Eq. (1.6).
Although the proof was made for the 2D OCP with a positive integer, it is reasonable to extend its validity to all real coupling values , within the fluid regime.
6 Conclusion
This work was motivated by the recent paper of Ferrero and Téllez Ferrero14 about the finitesize expansion of the grand potential for the 2D TCP at the coupling , in the presence of the impurity. The modification of the universal logarithmic term to the nonuniversal one, dependent on the charge of impurity, was there in agreement with the prediction (1.5) of nonneutral conformal field theories.
In this paper, we tested the prediction (1.5) of conformal field theory on the nonneutral 2D OCP. At the freefermion coupling (Sect. 4), we reproduce the result (1.5). Using the mapping of the 2D OCP onto the anticommuting field theory formulated on the chain, we were able to extend the finitesize analysis to an arbitrary coupling constant . This is one of rare occasions when the exact results are obtained for a series of pairinteger values. The nonuniversal prediction of conformal field theory (1.6) is confirmed as well.
It would be interesting to generalize our results to the 2D TCP or even to Coulomb fluids with an arbitrary charge composition. For such systems, we miss techniques analogous to that for 2D OCP, but a phenomenological approach might reveal the general form of the finitesize logarithmic term.
This work might be a further motivation for specialists to use Coulomb fluids as practical realizations of conformal field theories to test their predictions.
Acknowledgements.
The support received from Grant VEGA No. 2/0015/15 is acknowledged.References
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