Schwinger model simulations with dynamical overlap fermions

# Schwinger model simulations with dynamical overlap fermions

Wolfgang Bietenholz
NIC/DESY Zeuthen, Platanenallee 6
D-15738 Zeuthen, Germany
E-mail: bietenho@ifh.de
Speaker.
Stanislav Shcheredin
Fakultät für Physik, Univerisität Bielefeld
D-33615 Bielefeld, Germany
E-mail: shchered@physik.hu-berlin.de
Jan Volkholz
Institut für Physik, Humboldt-Universität zu Berlin
Newtonstr. 15, D-12489 Berlin, Germany
E-mail: volkholz@physik.hu-berlin.de
###### Abstract

We present simulation results for the 2-flavour Schwinger model with dynamical overlap fermions. In particular we apply the overlap hypercube operator at seven light fermion masses. In each case we collect sizable statistics in the topological sectors 0 and 1. Since the chiral condensate vanishes in the chiral limit, we observe densities for the microscopic Dirac spectrum, which have not been addressed yet by Random Matrix Theory (RMT). Nevertheless, by confronting the averages of the lowest eigenvalues in different topological sectors with chiral RMT in unitary ensemble we obtain — for the very light fermion masses — values for that follow closely the analytical predictions in the continuum.

Schwinger model simulations with dynamical overlap fermions

Jan Volkholz

Institut für Physik, Humboldt-Universität zu Berlin

Newtonstr. 15, D-12489 Berlin, Germany

E-mail: volkholz@physik.hu-berlin.de

\abstract@cs

The XXV International Symposium on Lattice Field Theory July 30 - August 4 2007 Regensburg, Germany

## 1 The Schwinger model

The Schwinger model [2] describes Dirac fermions in , interacting through a gauge field. In the Euclidean plane the Lagrangian reads

 \@fontswitchL(¯ψ,ψ,Aμ)=¯ψ(x)[γμ(i∂μ+gAμ)+m]ψ(x)+12Fμν(x)Fμν(x) . (1.0)

This is a popular toy model for QCD — for instance it is endowed with confinement. As a qualitative difference, however, there is no spontaneous chiral symmetry breaking. For degenerate flavours of mass the chiral condensate is given by111For the non-vanishing value originates from an axial anomaly and therefore from explicit chiral symmetry breaking (hence there is no contradiction to the Mermin-Wagner theorem).

 Σ(m)≡−⟨¯ψψ⟩∝(mNf−1β)1/(Nf+1)(β=1/g2) . (1.0)

Here we consider . In this case, there are analytical evaluations (using low energy assumptions) for the above proportionality constant in the case of light fermions (),

 \specialhtml:\specialhtml:Σ(m)={0.372 (m/β)1/3\@@cite[cite][\@@bibrefHHI]0.388 (m/β)1/3\@@cite[cite][\@@bibrefSmilga] (1.0)

## 2 Lattice formulation

We investigate the lattice formulation with compact link variables , and with the plaquette gauge action. For the fermions we employ an overlap hypercube fermion (overlap-HF) Dirac operator of the form (in lattice units)

 DovHF(m)=(1−m2)D(0)ovHF+m ,D(0)ovHF=1+(DHF−1)/√(D†HF−1)(DHF−1) . (2.0)

obeys the (simplest) Ginsparg-Wilson relation. Unlike the standard overlap operator with a Wilson kernel [5], we insert the truncated perfect hypercube fermion operator [6]. It involves couplings to nearest neighbour sites, and over plaquette diagonals (in the latter case gauging averages over the shortest lattice paths). By construction this kernel is approximately chiral already, and the overlap formula amounts to a correction that renders chirality exact.222To be precise, we use the chirally-optimised hypercube fermion (CO-HF) of Ref. [7]. This is optimal for our algorithm to be described in Section 3.

The overlap-HF has been applied in quenched QCD [8], and the HF was also used dynamically in finite temperature QCD [9]. In the 2-flavour Schwinger model has been first simulated with quenched re-weighted configurations [7, 10]. Compared to the standard overlap operator there is some computational overhead in the kernel, but has the following virtues [7]:

• Faster convergence in the polynomial evaluation of . Moreover the limitation to the use of low polynomials also improves the numerical stability.

• Higher degree of locality and approximate rotation symmetry.

• Improved scaling behaviour.

All these virtues are based on the similarity of the kernel to the overlap operator [6],

 \specialhtml:\specialhtml:DovHF≈DHF . (2.0)

## 3 The simulation

Here we report on HMC simulations, which are also facilitated by the property (2). Our algorithmic concept follows the simplified HMC force for improved staggered fermions of the HF-type [11]. The fermionic force of the standard HMC algorithm

 ¯ψQ−1ovHF[Q−1ovHF∂QovHF∂Ax,μ+∂QovHF∂Ax,μQ−1ovHF]Q−1ovHFψ , (3.0)

with the Hermitian operator , is simplified to

 (3.0)

approximates to a moderate (absolute) precision of . This approximation is useful and cheap thanks to relation (2) (which does not apply for the standard overlap operator). The Metropolis accept/reject step uses to machine precision (), which renders the algorithm exact. Our first experience at on a lattice, with trajectory length , was reported in Ref. [12]. Applying the Sexton-Weingarten integration scheme [13], we have meanwhile a compelling confirmation of acceptance rates in the range for the masses . Acceptance rates for the special case were also given in Ref. [14]. Our results show a remarkable stability in down to very light fermions. This holds for the total computing effort as well; note that the magnitude of the leading non-zero Dirac eigenvalue stabilises due to the finite size. In Ref. [12] we demonstrated that reversibility holds to a good precision. The degree of locality is stable in and strongly improved, even compared to the free standard overlap fermion, where the couplings decay as ( being the taxi driver distance between source and sink). For the free overlap-HF this decay is accelerated to . At it slows down only slightly to , with hardly any dependence on the masses that we investigated [12].

## 4 Results

In view of the -regime, we simulated at 7 fermion masses and collected data in the sectors with topological charge and (index of ). The corresponding statistics and the mean values of the leading non-zero eigenvalue of the Dirac operator —  stereographically projected onto a line —  are given in Table 1.

Chiral RMT has been worked out for the case of a non-vanishing chiral condensate in the chiral limit. This yields predictions for the low lying Dirac eigenvalues [17] in the -regime, which apply well in QCD [15, 16]. We show in Figure 1 the measured cumulative densities in our case, in the topologically trivial sector. This is compared to the RMT predictions for the parameters we are using (we refer to the unitary ensemble; the corresponding formulae are summarised in the second work quoted in Ref. [16]). They converge in terms of the dimensionless rescaled eigenvalue for very light or very heavy masses, where the latter limit corresponds to the quenched case. In the chiral limit this is obviously inapplicable in our situation. The plot in Figure 1 on the right also shows that the shape of the density for at finite mass does not match the RMT predictions. Instead we see a stabilisation in the eigenvalue itself (in a fixed volume ).

In this setting a total density is consistent with eq. (1) [18], and we can approximately confirm this behaviour, see Figure 2. The exponent is not singled out very precisely, but the essential observation is the absence of a Banks-Casher type plateau in the total eigenvalue density near 0.

Nevertheless, we observed an amazing connection to chiral RMT with respect to the ratio of in the sectors with topological charge and . We illustrated in Ref. [12] the chiral condensate as a function of this ratio at various masses, according to chiral Random Matrix Theory [17]. The combination of this RMT relation with in eq. (1) enables us to eliminate the chiral condensate and to arrive at a prediction for the ratio

 ⟨λ1,|ν|=1⟩⟨λ1,ν=0⟩(m) ,

which can be directly confronted with the numerical data in Table 1, see Figure 3.

The simulation results reveal a significant dynamical effect. For masses we take a step towards the -regime behaviour (insensitivity to ) and the condition is not on solid grounds anymore. But for the data match the predictions remarkably well (at very light masses the measured ratio tends to be just slightly above the prediction), although the latter combines apparently incompatible ingredients from chiral RMT the -regime and from infinite volume. This result can be compared to a study using quenched re-weighted configurations with the standard overlap operator [19]: that study obtained and a behaviour consistent with at large masses, but the proportionality constant was not reproduced and the proportionality could not be observed at small masses. In our case, Figure 3 is sensitive to both, the exponent and the proportionality constant in eq. (1), and both are confirmed well.

## 5 Conclusions

The overlap hypercube fermion has some computational overhead compared to the standard overlap fermion, but a number of benefits: better locality, approximate rotation symmetry, improved scaling and the applicability of a simplified HMC force. The restriction to low polynomials is particularly favourable for the numerical stability.

In our application to the 2-flavour Schwinger model on a lattice at we obtain useful acceptance rates and reliable reversibility. We cumulated statistics at masses and in the sectors of topological charge and 1 . We revealed a new type of microscopic Dirac spectrum, which is not explored analytically. Nevertheless, by combining RMT formulae for the spectrum with analytical expressions for , we obtained a prediction for the mass dependence of the ratio , which matches our numerical data at impressively well.

## A Testing the dynamical overlap-HF in QCD

We also implemented the HMC algorithm for in QCD, with the HF force which can be chirally corrected with Zolotarev polynomials of any degree . We display thermalisation histories of the dynamical overlap-HF in QCD, on lattices with polynomial degrees and . They are applied to the HMC force in the spectral interval with a lower bound or ( is the maximal Hermitian eigenvalue). For the precision parameter in eq. (3) we chose , the trajectory length now amounts to , and the accept/reject step is kept on machine precision.

At thermalisation sets in without problems (see Figure 4), whereas is plagued by a first order phase transition, which is further pronounced at (Figure 5).

Acknowledgement : We are indebted to Poul Damgaard, Stephan Dürr, Martin Hasenbusch, Urs Heller, Jacques Verbaarschot and Tilo Wettig for helpful discussions. J.V. was supported by the “Deutsche Forschungsgemeinschaft” (DFG). The computations were performed on the p690 clusters of the “Norddeutscher Verbund für Hoch- und Höchstleistungsrechnen” (HLRN).

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