Dirac-mode analysis for quark number density and its application for deconfinement transition

# Dirac-mode analysis for quark number density and its application for deconfinement transition

Takahiro M. Doi Speaker. T.M.D. is supported by the Grantin-Aid for JSPS fellows (No.15J02108) and the RIKEN Special Postdoctoral Researchers Program. e-mail: takahiro.doi.gj@riken.jp    Kouji Kashiwa
###### Abstract

The quark number density at finite imaginary chemical potential is investigated in the lattice QCD using the Dirac-mode expansion. We find the analytical formula of the quark number density in terms of the Polyakov loop in the large quark mass regime. On the other hand, in the small quark mass region, the quark number density is investigated by using the quenched lattice QCD simulation. The quark number density is found to strongly depend on the low-lying Dirac modes while its sign does not change. This result leads to that the quark number holonomy is not sensitive to the low-lying Dirac modes. We discuss the confinement-deconfinement transition from the property of the quark number density and the quark number holonomy.

Dirac-mode analysis for quark number density and its application for deconfinement transition

Takahiro M. DoiSpeaker. T.M.D. is supported by the Grantin-Aid for JSPS fellows (No.15J02108) and the RIKEN Special Postdoctoral Researchers Program. e-mail: takahiro.doi.gj@riken.jp and Kouji Kashiwa

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1Theoretical Research Division, Nishina Center, RIKEN, Wako 351-0198, Japan
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2Yukawa Institute for Theoretical Physics, Kyoto University, Kyoto 606-8502, Japan

• Abstract.

## 1 Introduction

One of the important task in nuclear and particle physics is the nonperturbative understanding of the phase structure of Quantum Chromodynamics (QCD) at finite temperature () and real chemical potential . However, the confinement-deconfinement transition has not been fully understood yet. For example, we cannot find any order parameter of the deconfinement transition in the case with dynamical quarks

The chiral and confinement-deconfinement transitions are key phenomena for this purpose, but the confinement-deconfinement transition is not yet fully understood comparing with the chiral transition. Although the chiral transition can be described by the spontaneous breaking of the chiral symmetry, but we can not find any classical order-parameters of the confinement-deconfinement transition in the presence of dynamical quarks.

The Polyakov loop, which respect the gauge-invariant holonomy, is the exact order-parameter of the confinement-deconfinement transition in the infinite quark mass limit. However, it is no longer the order parameter in the presence of dynamical quarks. Although other candidates for the order parameter of the deconfinement transition have been proposed  [1, 2, 3, 4, 5, 6], they are also not the exact order parameter. Therefore, we need some extension of ordinary determinations to clearly discuss and investigate the confinement-deconfinement transition in the system with dynamical quarks.

Recently, in Refs. [7, 8, 9], it is found that the topological change of QCD thermodynamics at finite can be used to determine the confinement-deconfinement transition, and based on the non-trivial free-energy degeneracy, the quark number holonomy which is defined by the contour integral of the quark-number susceptibility of has been proposed as the quantum order-parameter for the confinement-deconfinement transition. This argument is based on the analogy of the topological order discussed in Refs. [10] and QCD at  [11] in the condensed matter physics. The quark number holonomy counts the gapped points of the quark number density along . As a results, it becomes non-zero/zero in the deconfined/confined phase. In particular, the quark number density at is important because it gives the property of the quark number holonomy. In order to investigate the quark number density at , we use the Dirac-mode expansion [12]. And we will see the behavior of the quark number density by removal of the low-lying Dirac modes.

This paper is organized as follows. In the section 2, we show the heavy quark mass expansion of the quark number density. In the section 3, we discuss the Dirac-mode expansion of the quark number density in both large and small quark mass regime. Section 4 is devoted to summary and discussions.

## 2 large-mass expansion of quark number density

In this study, we consider the lattice QCD on the standard square lattice. We denote each sites as and link-variables as . We impose the temporal periodic boundary condition for link-variables to generate configurations in the quenched calculation to manifest the imaginary-time formalism.

On the lattice, the quark number density is defined as

 nq=1V∑x⟨¯q(x)∂D∂μq(x)⟩=1V⟨Trγ,c[∂D∂μ1D+m]⟩, (1)

where denotes the functional trace and is taken over spinor and color indices. The Dirac operator in this article is taken as the Wilson-Dirac operator with quark mass and the chemical potential in the lattice unit as

 D=−123∑k=1[P(+k)^Uk+P(−k)^U−k]−12[eμP(+4)^U4+e−μP(−4)^U−4]+4⋅^1, (2)

where is the identity matrix. The link-variable operator is defined by the matrix element

 ⟨x|^U±ν|x′⟩=U±ν(x)δx±^ν,x′, (3)

with and with . The chemical potential is the dimensionless on the lattice and we define .

We impose the temporal anti-periodicity and spatial periodicity for . To that end, we add a minus sign to the matrix element of the temporal link-variable operator at the temporal boundary of :

 ⟨x,N4|^U4|x,1⟩=−U4(x,N4),       ⟨x,1|^U−4|x,N4⟩=−U−4(x,1)=−U†4(x,Nt). (4)

In this notation, the Polyakov loop is expressed as

 L≡1NcV∑xtrc{N4−1∏n=0U4(x+n^4)}=−1NcVTrc{^UN44}. (5)

The minus sign stems from the additional minus on in Eq.(4).

In the heavy quark mass region, the quark number density (1) can be expressed by using the quark mass expansion as

 nq=1MV⟨Trγ,c[∂D∂μ∞∑n=0(−^DM)n]⟩≡1MV∞∑n=0c(n)(−M)n, (6)

where we define the effective mass and the operator . In the case of the large quark mass, with smaller are dominant. The -th order contribution has the terms

 c(n)=c(n)1+c(n)2+c(n)3+⋯, (7)

and is a product of link-variables. The examples of the paths of the products are shown in Fig. 1. Note that many of them become exactly zero because of Elitzur’s theorem [13]; only the gauge-invariant terms corresponding to closed loops are nonzero. Moreover, spatially closed loops which do not wind the temporal length are canceled out each other and have no contribution to the quark number density in total in each order . Noting these important facts, it is confirmed that the -th order contribution is constituted of the gauge-invariant loops with the length which winds the temporal direction. In particular, the nonzero leading term in the expansion (6) is the -th order term which relates to the Polyakov loop () and its complex conjugate (). The leading term, , to the quark number density at finite is written as

 c(N4−1)∼eiθL−e−iθL∗=2sin(θ+ϕ)|L|. (8)

In the heavy quark-mass expansion of the quark number density (6), there are higher order terms beyond the leading terms, which are the Polyakov loop and its conjugate. By similar analysis in the case of the leading term, the higher-order terms can be expressed in terms of the quantities which correspond to loops on the lattice. For example, the sub-leading terms include a term proportional to the quantity

 c(N4+1)1≡Trc{^U4U1U4U−1UN4−24}. (9)

These terms correspond to the closed paths which wind the temporal length and bypasses the spatial direction. As another example, loops winding the temporal direction twice or more can be contribute to the expansion (6). For example, a loop winding the temporal direction twice

 c(2N4−1)1≡Trc{^U2N44} (10)

is a possible contribution to Eq. (6) as the ()-th order term.

## 3 Dirac-mode expansion of the quark number density

In the following, we consider the quark number density in terms of the Dirac eigenmode. In large quark mass region, we analytically investigate it in all order of the large quark mass expansion (6). In small quark mass region, we perform the quenched lattice QCD simulation.

The Wilson-Dirac eigenvalues are obtained from the eigenvalue equation as

 D|n⟩=λn|n⟩, (11)

where is the Wilson-Dirac eigenstate. Considering the Wilson-Dirac mode expansion of the chiral condensate, the low-lying eigenmodes of the operators have dominant contribution to the chiral condensate known as Banks-Casher relation [14, 15].

### 3.1 large quark mass region

We start the leading term to express it in terms of the Wilson-Dirac modes. The leading contribution of the quark number density in large quark mass region (8) is expressed by the Polyakov loop and its complex conjugate. It is already known that the Polyakov loop can be expressed in terms of the eigenmodes of the naive-Dirac operator which corresponds to the case of [16, 17] and the Wilson-Dirac operator [18, 19]. In the following, we derive a different form of the Dirac spectral representation of the Polyakov loop using the operator on the square lattice with the normal non-twisted periodic boundary condition for link-variables, in both temporal and spatial directions. We define a key quantity,

 I(N4−1)=Trc,γ(D^UN4−14). (12)

This quantity is defined as the slightly changed quantity from the Polyakov loop by replacing a temporal link-variable to the Wilson-Dirac operator . This quantity can be calculated as

 I(N4−1)=2e−μNcVL. (13)

Thus, the quantity is proportional to . Here, other terms vanish because of the Elitzur’s theorem and the trace over the Dirac indecies. On the other hand, since in Eq. (12) is defined through the functional trace, it can be expressed in the basis of Dirac eigenmodes as

 I(N4−1)=∑n⟨n|D^UN4−14|n⟩+O(a)=∑nΛn⟨n|^UN4−14|n⟩+O(a). (14)

The term arises because Wilson-Dirac operator is not normal due to the Wilson term and the completeness of the Wilson-Dirac eigenstates has the error:

 ∑n|n⟩⟨n|=1+O(a). (15)

However, this error is controllable and can be ignored in close to the continuum limit.

Combining Eqs. (13) and (14), one can derive the relation between and the Dirac modes as

 L≃e−μ2NcV∑nΛn⟨n|^UN4−14|n⟩, (16)

with the error. From the formula (16), it is analytically found that the low-lying Dirac modes with have negligible contribution to the Polyakov loop because the eigenvalue plays as the damping factor. It is also numerically shown that there is no dominant contribution in the Dirac modes to the Polyakov loop [17]. Thus, one can find the Dirac spectrum representation of the quark number density in the leading order and the low-lying Dirac modes have little contribution to the quark number density.

The above discussion on the leading term can be applicable to the Dirac spectrum representation of the higher order terms. The detailed discussion is shown in our recent paper [20]. In the same way in the case of the leading term, all the terms in the expansion (6) can be expressed in terms of the Wilson-Dirac modes. Thus, it is analytically found that the quark number density does not depend on the density of the low-lying Wilson-Dirac modes in the all-order. However, this fact is only valid in the sufficiently large quark mass region since other contributions which can not be expressed by and can appear in the small region.

### 3.2 Small quark mass region

Next, we consider the small mass regime. In this regime, we perform the lattice QCD simulation to investigate the quark number density. In this study, we perform the quenched calculation with the ordinary plaquette action and then fermionic observables are evaluated by using the Wilson-Dirac operator (2) with the imaginary chemical potential . Our calculation is performed in both the confinement phase and the deconfinement phase. In the confinement phase, we consider lattice with and which corresponds to fm and MeV. In the deconfinement phase, we consider lattice with and which corresponds to fm and MeV. Both values of correspond to . In both cases, we set the quark mass as in the lattice unit, which is equivalent to the hopping parameter , for the calculation of the eigenmodes of the Wilson-Dirac operator in the small quark mass region [21].

We calculate the quark number density as

 ⟨nq⟩=12V⟨Trγ,c[∂D∂μ1D+m−(∂D∂μ1D+m)†]⟩≃iVIm⟨∑n⟨n∣∣∂D∂μ∣∣n⟩1Λn+m⟩. (17)

This form trivially takes pure imaginary value up to the error. Each contribution, , to the quark number density of the Dirac mode with can be defined as

 nnq=iVIm⟨n∣∣∂D∂μ∣∣n⟩1Λn+m, (18)

and then the quark number density becomes

 nq=∑nnnq. (19)

In Fig. 3, is shown in the cases with and . We here only show results with one particular configuration.

To investigate the quark number density in terms of Dirac modes, we define the infra-red (IR) cutted quark number density with the cutoff as

 ncutq(ΛIR)=1nq∑|Λn|>ΛIRnnq. (20)

In Fig. 4, we shown the result at , where the system is in the deconfinement phase. In general, we can perform the configuration average in the evaluation of Eq. (20). However, since the averaging well works after summing over all Dirac-modes, it misses a physical meaning. Then, we show in one particular configuration.

Note that the sign of the quark number density does not changed by removing the low-lying Dirac modes while the absolute value of the quark number density seems to drastically change. This tendency has been found in almost all our configurations. This result means that the absolute value of the quark number density shares a same property in terms of Dirac modes with the chiral condensate, while its sign shares the property with the Polyakov loop.

Finally, the topological confinement-deconfinement transition can be discussed in terms of the Dirac-mode analysis. The order-parameter of the topological confinement-deconfinement transition can be expressed [8] as

 Ψ =∮2π0{Im(d~nqdθ∣∣T)}\leavevmode\nobreak dθ, (21)

where is the dimensionless quark number density such as . It counts gapped points of the quark number density along direction and thus it becomes zero/non-zero in the confined/deconfined phase. The quark number holonomy (21) can be expressed as

 Ψ =±2Nclimϵ→0[Im\leavevmode\nobreak ~nq(θ=θRW∓ϵ)], (22)

when the RW endpoint which is the endpoint of the RW transition line becomes the second-order point at . In Eq. (22), characterizes and thus shares the same property about the Dirac modes with . The important point here is that the absolute value of does not have so much meaning even if it is non-zero, but its sign is important since the sign flipping at characterizes the gapped points along -direction. From our quenched lattice QCD data, the sign of the quark number density are insensitive to the low-lying Dirac-modes and this behavior is similar to the Polyakov loop.

## 4 Summary and discussion

In this paper, we have discussed properties of the quark number density at finite temperature () and imaginary chemical potential () by using the Dirac-mode expansion.

From the heavy quark mass expansion with the Dirac mode expansion, we found that low-lying Dirac modes do not dominantly contribute to the quark number density in all order of the heavy quark mass expansion.

In the small quark mass regime, we found that the absolute value of the quark number density strongly depends on low-lying Dirac modes, but its sign does not. Our result shows that the quark number holonomy is sensitive to the confinement properties of QCD and it is the good quantum order parameter for the confinement-deconfinement transition.

In order to avoid the incompleteness of the Wilson-Dirac modes, one can consider the hermitian Wilson-Dirac operator . In fact, the actual calculation is shown in our recent paper [20]. Moreover, the more detailed calculation on the higher order terms in the large-mass expansion is also included in it.

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