научная статья по теме DYNAMICAL SYMMETRY BREAKING IN MODELS WITH THE YUKAWA INTERACTION Физика

Текст научной статьи на тему «DYNAMICAL SYMMETRY BREAKING IN MODELS WITH THE YUKAWA INTERACTION»

ЯДЕРНАЯ ФИЗИКА, 2013, том 76, № 4, с. 572-574

= ЭЛЕМЕНТАРНЫЕ ЧАСТИЦЫ И ПОЛЯ

DYNAMICAL SYMMETRY BREAKING IN MODELS WITH THE YUKAWA INTERACTION

©2013 V. G. Ksenzov1), A. I. Romanov2)

Received April 25, 2012; in final form, June 22, 2012

The models with a massless fermion and a self-interacting massive scalar field with the Yukawa interaction are discussed. The chiral condensate and the fermion mass are calculated analytically through a one-loop approximation in (1 + 1)-dimensions. It is shown that the models have a phase transition as a function of the squared mass of the scalar field.

DOI: 10.7868/S004400271302013X

The dynamical chiral symmetry breaking (DCSB) plays an important role in attempts to describe different physical phenomena in the realm of elementary particles. That is why much attention has been attracted to the investigation of DCSB in different models ([1—8] and references therein).

In the first paper on this subject [1], Nambu and Jona-Lasinio (NJL) analyzed a specific field model in four dimensions. Later, DCSB was studied [2] by Gross and Neveu (GN) in a (1 + 1)-dimensional space—time in the limit of a large number of fermion flavors N. These two models are similar but, in contrast to the NJL model, the GN model is a renor-malizable and asymptotically free theory. Due to these properties, the Gn models are used for qualitative modeling of QCD at finite temperature and hadron density (see, e.g., [3] and references therein). The relative simplicity of both models is a consequence of the quartic fermion interaction. In a real situation, the chiral condensate is obtained by numerical studies, especially via lattice simulations [6]. In these calculations the Bank—Casher formula is often used [8].

In the present paper we study a system of a self-interacting massive scalar and a massless fermion field with the Yukawa interaction. In a (1 + 1)-dimensional space—time and in the limit of a large mass of the scalar field, our model becomes equivalent to the GN model.

The studied model has a discrete symmetry that can be broken either through the mechanism of the spontaneous symmetry breaking at classical level (SSBCl), i.e., by the potential U(4>) Eq. (1) (see below) without quantum corrections (if the scalar

1)State Scientific Center Institute for Theoretical and Experimental Physics, Moscow, Russia.

2)National Research Nuclear University MEPhI, Moscow, Russia.

sector makes this possible) or dynamically by means of DCSB. The latter is characterized by the chiral condensate {ipl), which plays the role of an order parameter. To obtain a general analytic expression for the chiral condensate, we employ the functional integral method, as described below. We find that the chiral condensate is equal to zero when the scalar field develops a nonzero vacuum expectation value by means of the SSBCl mechanism. When there is no SSBCl mechanism, the discrete symmetry is broken dynamically by the chiral condensate. Therefore we conclude that this model has a phase transition as a function of the mass of the scalar field squared [9].

We consider a model with the Lagrangian density which is given by

L = Lb + Lf = ^{d^)2-U{<P)+ (1) + ipa/1a -

where 0(x) is a real scalar field, 1a(x) is a massless fermion field and the index a runs from 1 to N (N » » 1). The potential of the scalar field,

U{<t>) = l-m2<t>2 + V{<t>2),

includes the mass term and the self-interaction V(rf>2) of the scalar field.

Lagrangian (1) is invariant under the discrete transformation

1a ^ Y51a, P ^-p75, 0 (2)

The symmetry of Eq. (2) can be broken either through the SSBCl mechanism or by the chiral condensate. In order to see how these two possibilities are realized, we need to calculate the chiral condensate in the model (1).

DYNAMICAL SYMMETRY BREAKING

573

The chiral condensate is given by the functional integral

g? r) = (3)

^¡DtDPDr&r*™-,

where Z is a normalization constant and n is the spacetime dimension. Equation (3) can be rewritten as

= 4 [ Dfc* J Lb(x)<F,(x) x

Z

(4)

It should be noted that the accuracy of Eq. (9) is determined by that of the stationary phase approximation. One can see from Eq. (9) that the chiral condensate is equal to zero when the scalar field obtains a vacuum expectation value through the SSBCl mechanism because in this case the classical potential U(0) has a minimum at 0 = 0m.

In order to study the properties of the chiral condensate, we need to choose a specific potential of the scalar field. We take the potential U(0) as

S

aJjLf (x)dn(x)

x i— I DfDfe'

J

Integrating by parts [10], we obtain

(Q\gtpa ^a |Q) =

Щф) = ±т2ф2 + ±ф*.

(10)

(5)

The fermionic Lagrangian is purely quadratic in the fields and we can therefore integrate over them, getting

In the following, we limit the consideration to the case of n = (1 + 1)-dimensional space—time. In this case constants g and A are dimensional, and it is convenient to introduce dimensionless coupling constants

n - 9 \ - A

go — —, a0 — —o • m m2

Rescaling the scalar field as 0(x) = m0(x) (and omitting the bar in the rescaled field), we rewrite the effective action (7) as

(0\дфа фа |Q) =

(6)

±/пф($Ф + ±и(ф) )e

,2 a, d TT/A\ \ JS

S=J

m2 4!

d2x — iN tr ln(i/ — д0ф).

(11)

where the effective action S is

S = J Lb{x)dnx - гЖгЫ{гф - дф). (7) фт + + N

The stationary point is given by the solutions of

2a „2A2

Ac J 3 I AT goф m ^ %Ф m

Q, (12)

We calculate the chiral condensate using the method of the stationary phase. A minimum of the effective action of the system can be reached if the effective potential and kinetic energy are minimal each on its own:

6m2 m 2n A2 where A is the ultraviolet cutoff.

Using potential (10), the chiral condensate (9) becomes

— (Q\gc Г фа\0) = фт +

Хо-ф3 m

(13)

ией(ф) = min and д^ф = Q,

(8)

where

J Ueff(0Kx = J U(0)dnx + iNtrln(i/ - g4>).

Let the constant scalar field satisfy condition (8). We take into account the constant scalar field because the chiral condensate is a constant, therefore

in Eq. (9) must be a constant as well.

^ , 6m2rm-

Since the chiral condensate (13) is expressed in terms of odd powers the sign of the condensate is defined by the sign of

To investigate the properties of the chiral condensate we consider the following two possibilities: (i) Ao = Q. In this case the solutions of Eq. (12) are

dU(<f>)

<1ф

доф2т = Л exP ( —

2тг 9ÎN

Ф=Фт

That is possible if 0m is a constant, which must satisfy Eq. (8). The factor in front of the exponent in Eq. (6) is fixed at the point 0 = 0m, which allows to evaluate the integral, one obtains

and, introducing

gc фт = = ±Лехр ( —

П

gCN

d

(0\дфафа\0) = - —и{ф)

(9)

we get the chiral condensates (9) as

(Q\g2^a\Q) =

±

Ф=Фт

(14)

(15)

ЯДЕРНАЯ ФИЗИКА том 76 №4 2013

574

KSENZOV, ROMANOV

This expression reproduces the result of [2]. Here, we multiply on g0 the chiral condensate to obtain a renormalization invariant quantity. Indeed, the GN model is asymptotically free and the f3 function in one-loop approximation is [2]

R(n \ — \ dg° - g°N

(16)

Using (16), one can verify that x— does not depend on the choice of renormalization point, so the fermionic mass ¡f = = go0m is a meaningful physical quantity. If we change the sign in front of the 02 term in Eq. (11), we get

9o0m = /4 = ±Aexp (j^j ■ (17)

In this case the scalar field is a tachyon and the fermionic mass is not a renormalization invariant quantity. In the limit A2 ^ to, the fermionic mass becomes infinity as well. In both cases the fermionic mass is a nonperturbative quantity.

(ii) Ao =0. In this case Eq. (12) becomes

2^2 m

6m2 2vr /x2

0.

(18)

This equation does not admit analytic solutions for an arbitrary Ao. We will consider Ao/g"^N < 1, in which case one can solve Eq. (18) by perturbing around

0m = 00':

= 00 +

Ao

920N

V.

(19)

Here, 0o is a solution of Eq. (12) corresponding to A0 = 0. Substituting (19) in (18), we get

n

V

6 m2^

(20)

0m =

1

n

Ao

6m2 g0N '

Then from (13) the chiral condensate is given by

-(og rr\o) = (21)

+ i Ao = H--

6m2g0

1

n

go2N

(j+)

+3

Here, the solution j— was chosen for a definiteness. The fermionic mass in this case yields

One can see that the scalar field potential destroys the renormalization invariance of the fermionic mass (22).

jf = go0m = 1 -

For a tachyonic scalar field 0 (m2 < 0) the fermionic mass must be obtained by the SSBCl mechanism, because the chiral condensate is zero. Finally, we can see that the chiral condensate depends on the sign of m2: there is a condensate for positive m2 but not for negative m2. We conclude that this model has a phase transition as a function of m2. A phase transition of this kind was discussed in [9].

To summarize, in this paper we studied dynamical chiral symmetry breaking in a model which consists of a fermion field and a self-interacting scalar field, with the Yukawa interaction between the two fields. In our model, the discrete chiral symmetry can be broken either by the SSBCl mechanism or dynamically by a nonzero chiral condensate. It was shown that the presence of the SSBCl mechanism does not allow for a nonzero chiral condensate. We further constrained the study to a (1 + 1)-dimensional space—time and in the limit of large N. Also, the self-interaction of the scalar field was assumed to be treatable as perturbation. In this case analytic expressions for the chiral condensate and the fermionic mass have been obtained. We conclude that the model considered has a phase transition as function of m2, since the chiral condensate is equal to zero in the SSBCl case (m2 < 0) and is not zero in the case m2 > 0. The method proposed here makes it possible to calculate the chiral condensate for various scalar potentials and for arbitrary space—time dimensions.

We are grateful to O.V. Kancheli, A.E. Kudryavt-sev, Y.M. Makeenko, V.A. Lensky, and M.A. Zubkov for stimulating discussions.

REFERENCES

1. Y. Nambu and G. Jona-Lasinio, Phys. Rev. 122, 345 (1961).

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