Lattice simulation of SU(2) gauge theory with chirally symmetric fermions

Lattice simulation of SU(2) gauge theory with chirally symmetric fermions

Abstract

We numerically study the SU(2) gauge theory with two dynamical flavors of the domain-wall fermions in fundamental representation. The meson spectra and the residual mass are measured on three lattice volumes and at two values of gauge coupling so as to investigate the finite volume effect. On generated configurations, eigenvalues of the overlap fermion operator are determined and compared to the random matrix theory. To quantify the effect of violation of the exact chiral symmetry, we measure the correlation between the eigenvectors of the domain-wall and the overlap operators.

\ShortTitle

Lattice simulation of SU(2) gauge theory with chirally symmetric fermions \FullConference 31st International Symposium on Lattice Field Theory LATTICE 2013
July 29 - August 3, 2013
Mainz, Germany

1 Introduction

The SU(2) gauge theory has for long time been studied as a prototype theory of QCD that shares important features with QCD such as chiral symmetry breaking and confinement, while with less numerical cost. Recently it has been drawn much attention in search for a theory beyond the standard model as a candidate of technicolor theory [1, 2, 3, 4]. In this work, we also focus on the chiral dynamics of SU(2) gauge theory. The pattern of spontaneous chiral symmetry breaking depends on the gauge group and the fermion representation. QCD, and in general SU() with gauge theory with fundamental fermions are considered to chirally break down as , where is the number of flavors. Since SU(2) group is pseudoreal, it has a pattern of chiral symmetry breaking different from QCD: SU(2)Sp(2). The adjoint representation of fermions results in another pattern SU(2)SO(2) for any . One of the motivations of this work is to understand the effect of the symmetry breaking pattern on the chiral dynamics, in particular its dependence on the number of flavors and temperature.

To explore the chiral symmetry on the lattice, it is important to employ the fermion formulation that retains the chiral symmetry as exact as possible. In this sense, the overlap fermion operator,

(1)

is the best solution, where is the Hermitian Wilson-Dirac operator with the domain-wall height. satisfies the Ginsparg-Wilson relation, which expresses an exact chiral symmetry on the lattice. In particular, simulations in the so-called -regime are an attractive device to extract the chiral condensate precisely. However, its numerical cost is high and to reduce it down to an acceptable level, elaborated setup, such as reduction of near-zero modes of by employing the topology fixing term, is demanded. Such situation may cause the simulation and analysis involved.

An alternative approach is the domain-wall (DW) fermion. The DW fermion operator is defined as a massive fermion in the five-dimensional space, and light modes appear on the boundaries in the 5th dimension. The DW action is written as

(2)

where is fermion mass, , the size of 5th dimension, and the Wilson operator with negative mass,

(3)

Taking the limit of with fixed , the action (2) accompanied by Pauli-Villars ghost term arrives at the overlap fermion operator (1). How much the chiral symmetry is violated in DW fermion action is probed by a quantity

(4)

where

(5)

An average of over large separation is a standard definition of the residual mass.

Our original strategy is to explore the dynamics of the chiral symmetry breaking with the overlap fermion in the -regime in which the Compton wave length of the PS meson is larger than the system size [5]. The eigenvalue distribution of the overlap fermion can be compared to the chiral random matrix theory so as to extract the chiral condensate with high precision. However, due to aforementioned complication, we decided to perform first the dynamical simulations with DW fermions as a reference and for systematic survey.

In this paper, we focus on the SU(2) gauge theory with two flavors of fundamental domain-wall fermions, as a basis to investigate the dependence and the properties at finite temperature. The setup of numerical simulations is described in the next section. Sections 3 and 4 describe the results of measurement with valence domain-wall and overlap operators, respectively. How the eigenmodes of the former approach to the latter is discussed in Sec. 5. The last section is devoted to summary and outlook.

2 Simulation setup

Figure 1: -dependence of the lattice spacing defined through the Sommer’s hadronic radius for quenched and simulations with the Iwasaki gauge and the domain-wall fermion actions.

The gauge configurations are generated with the Iwasaki gauge action with dynamical fermions with the standard DW fermions accompanied by the Pauli-Villars ghosts. We employ the Hybrid Monte Carlo algorithm with the Omelyan integrator and multi-time-step. The code is implemented by modifying the Bridge++ code set [6] so as to enable SU(2) simulations. The lattice sizes are , , and . As the parameters of the DW fermions, we use , and throughout present work.

We first observe the -dependence of the lattice spacing. Although the lattice spacing in physical units does not make sense for the present theory, it is often convenient to draw a rough idea of the scale. Figure 1 displays the -dependence of the lattice spacing defined through the Sommer’s hadronic radius fm that was determined from the static fermion potential in the quenched and cases. Based on this result, we decided to adopt and 0.90 as our first target of numerical simulations. The mass of the dynamical domain-wall fermion is varied from to 0.20.

3 Meson spectrum and residual mass

We first measure the meson spectrum and the residual mass under variation of valence fermion mass. Using a local meson operator at both the source and sink, statistics of 20-40 configurations is sufficient to determine the PS meson masses, while not for the other channels. Figure 2 shows the volume dependence of the PS and V meson masses at and 0.90 with . The PS meson mass is proportional to the valence fermion mass, as is familiar in QCD. The finite intercept indicates the explicit breaking of the chiral symmetry in the DW fermion formulation. The offset values are consistent with the direct calculation of the residual mass with Eq. (4). While the values of the residual mass is not negligibly small, it decreases as increases as is expected.

Figure 2: The finite size effect on the masses of PS and V mesons at (left panel) and 0.90 (right) and the sea fermion mass .
Figure 3: Meson masses in PS, V, S and A channels for the valence fermion mass on 250 configurations generated at and the sea fermion mass on the lattice.

The left panel of Fig. 2 compares the meson masses in three volumes at . While the values for and are consistent, the result for is slightly larger. Extrapolating to , for and 3.6 for , and thus the above results are consistent with the wisdom in QCD that is required to avoid large finite volume effect. At displayed in the right panel of Fig. 2, only and cases have been obtained which are significantly deviate. Since for and 3.6 for , to settle the finite volume effect we need a result for that computation is now in progress.

Once the finite size effect and size of chiral symmetry breaking are quantified, we can systematically investigate the meson spectrum and other observables. For the channels other than PS and V, however, the correlators suffer from larger statistical fluctuation. In Figure 3 we show an example of meson masses on lattice at with higher statistics. By applying the same setup as PS and V mesons, configurations are not enough to extract the masses of S and A channels in sufficient precision. Some kind of techniques to increase the signal is necessary such as the all-to-all propagators.

4 Valence overlap fermion operator

It is interesting to measure the eigenmodes of the valence overlap fermion operator on the configurations generated with DW fermions. As numerical implementation of the overlap operator (1), we adopt the Zolotarev’s partial fractional approximation to the sign function with the low-mode projection of . The low-lying eigenmodes of massless are determined by applying the implicitly restarted Lanczos algorithm. Figure 4 shows an example of measurement on lattice at and . The left panel shows the distribution of the number of zero modes whose deviation give the topological susceptibility. The right panel shows the density of the low-lying eigenmodes. Clearly the result shows the expected behavior for the broken chiral symmetry through the Banks-Casher relation. Quantitative analysis is now underway.

Figure 4: The distribution of zero modes (left panel) and the density of low-lying eigenvalues (right) of the valence overlap fermion operator at and on lattice.

Once the distribution of the eigenvalues are determined, it can be compared to the prediction of the random matrix theory. In this context the most interesting quantity is the distribution of low-lying eigenvalues, that is to be compared with the chiral random matrix theory [7]. However, our present setup and statistics are not suitable to such an analysis. We instead compare the level statistics of the bulk region of the eigenvalue spectrum to the random matrix theory. It is not related to the chiral dynamics but just reflects the symmetry of the fermion operator.

Figure 5 shows the density of the unfolded level spacing at and 1. The unfolding is applied to the eigenmodes in the range [0.2,0.8] which are measured on 500 configurations irrespective to the topological charge. In the figure, predictions of the random matrix theory with three types of ensembles, orthogonal (GOE), unitary (GUE), and symplectic (GSE) are also displayed. The numerical result is well consistent with the GOE curve that corresponds to the symmetry of fundamental representation of SU(2) group.

Figure 5: Unfolded level spacing of the overlap fermion operator at and on lattice. The predictions of the random matrix theory for GOE, GUE, and GSE are also displayed.

5 Correlation between DW and overlap eigenmodes

Since the dynamics of the chiral symmetry breaking is encoded in the low-lying eigenmodes, these modes can be used to quantify the effect of chiral symmetry violation brought by adopting the domain-wall fermion action. The four-dimensional domain-wall operator [8, 9],

(6)

where , is the counterpart of the overlap operator that approaches Eq. (1) in the limit . Thus we investigate the correlation between the eigenvectors of Eq. (1) and of Eq. (6) determined on the same configurations.

Figure 6 displays the correlation of the 40 lowest eigenmodes of the 4D domain-wall and overlap fermion operators, , on single configuration. The left and right panels show the results at () and (), respectively. As expected, near-diagonal components of the correlation increase as the residual mass decreases. The same tendency is generally observed on other configurations, while a quantitative analysis is underway.

Figure 6: Correlation between the eigenmodes of the domain-wall and overlap operators. The left and right panels are at and 0.90, respectively.

6 Conclusion and outlook

We are investigating the SU(2) gauge theory with dynamical fermions in the fundamental representation. Numerical simulations with two-flavors of domain-wall fermions were performed as a basis for extensive studies with variation of number of flavors and at finite temperature. The results obtained are feasible for further investigation, while techniques to increase the signal is required for quantitative computation of variety of meson sectors. We also observed the eigenmodes of the valence overlap operator which is useful to explore the effect of the chiral symmetry violation of the domain-wall fermions. We are preparing for systematic studies of subjects described in this paper, as well as for applying the same procedure to the adjoint representation of fermions.

Acknowledgment

We thank S. M. Nishigaki for useful discussion and for analysis to generate Fig. 5. Numerical simulations were performed on Hitachi SR16000 and IBM Blue Gene/Q at KEK under a support of its Large-scale Simulation Program (No.12/13-15) and computer system at KMI, Nagoya University. We also thank the Japan Lattice Data Grid which is a grid file system constructed on a virtual private network SINET4 provided by National Institute of Informatics for efficient data transfer. This work is supported in part by the Grand-in-Aid for Scientific Research of the Japan (Nos.20105005, 22224003, 22740183, 25400284).

Footnotes

  1. This analysis was performed by S. M. Nishigaki.

References

  1. For reviews, E. T. Neil, PoS LATTICE 2011 (2011) 009 [arXiv:1205.4706 [hep-lat]]; J. Giedt, PoS LATTICE 2012 (2012) 006.
  2. R. Lewis, C. Pica and F. Sannino, Phys. Rev. D 85 (2012) 014504 [arXiv:1109.3513 [hep-ph]].
  3. T. Karavirta, J. Rantaharju, K. Rummukainen and K. Tuominen, JHEP 1205 (2012) 003 [arXiv:1111.4104 [hep-lat]].
  4. M. Hayakawa et al., Phys. Rev. D 88 (2013) 094504 [arXiv:1307.6997 [hep-lat]]; Phys. Rev. D 88 (2013) 094506 [arXiv:1307.6696 [hep-lat]].
  5. H. Matsufuru, Y. Kikukawa, K. -I. Nagai and N. Yamada, PoS LATTICE 2010 (2010) 090; H. Matsufuru, Y. Kikukawa and N. Yamada, PoS LAT 2009 (2009) 064.
  6. Bridge++ project website, http://bridge.kek.jp/Lattice-code/.
  7. P. H. Damgaard and S. M. Nishigaki, Phys. Rev. D 63 (2001) 045012 [hep-th/0006111].
  8. Y. Kikukawa and T. Noguchi, hep-lat/9902022.
  9. A. Borici, Nucl. Phys. Proc. Suppl. 83 (2000) 771 [hep-lat/9909057].
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