The repulsive core of the NN potential and the operator product expansion

The repulsive core of the NN potential and the operator product expansion

Sinya Aoki 
Graduate School of Pure and Applied Sciences, University of Tsukuba, Tsukuba, Ibaraki 305-8571, Japan
E-mail: saoki@het.ph.tsukuba.ac.jp
Speaker.
   Janos Balog
Research Institute for Particle and Nuclear Physics, 1523 Budapest 114, Pf. 49, Hungary
E-mail: balog@rmki.kfki.hu
   Peter Weisz
Max-Planck-Institut für Physik, Föringer Ring 6, D-80805 München, Germany
E-mail: pew@mppmu.mpg.de
Abstract

We investigate the short distance behavior of the nucleon–nucleon (NN) potential defined through the Bethe-Salpeter wave function, by perturbatively calculating anomalous dimensions of 6–quark operators in QCD. Thanks to the asymptotic freedom of QCD, the 1-loop estimations give exact results for the potential in the zero distance limit. We show that the chiral symmetry of the gauge interaction implies the existence of an operator whose anomalous dimension is zero for a given quantum number. Furthermore we find that non-zero anomalous dimensions of other operators are all negative. These results predict the functional form of the NN potential at short distance, which is a little weaker than . On the other hand, the computation of the anomalous dimension spectrum alone can not determine whether the potential is repulsive or attractive at short distance. An additional analytic non-perturbative analysis suggests that the force at short distance is indeed repulsive at low energy as found numerically. Some extensions of the method are briefly discussed.

The repulsive core of the NN potential and the operator product expansion

 

Peter Weisz

Max-Planck-Institut für Physik, Föringer Ring 6, D-80805 München, Germany

E-mail: pew@mppmu.mpg.de

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The XXVII International Symposium on Lattice Field Theory - LAT2009 July 26-31 2009 Peking University, Beijing, China

1 Introduction

In a recent paper [1], the nucleon-nucleon(NN) potentials have been calculated in lattice QCD from the Bethe-Salpeter (BS) wave function through the Schrödinger equation. The results qualitatively resemble phenomenological NN potentials which are widely used in nuclear physics. The force at medium to long distance ( fm) is shown to be attractive. This feature has long well been understood in terms of pion and other heavier meson exchanges. At short distance, a characteristic repulsive core is reproduced by the lattice QCD simulation [1]. No simple theoretical explanation, however, exists so far for the origin of the repulsive core.

A hint to understand the repulsive core theoretically has appeared in Ref.[2], where properties of the BS wave function of the Ising field theory in 2-dimensions,

(1.0)

are considered analytically. Here is the rapidity of the one particle state. From the operator product expansion (OPE)

(1.0)

the BS wave function at short distance becomes

(1.0)

which predicts the short distance behavior of the potential as

(1.0)

The OPE in this case predicts not only the behavior of the potential at short distance but also its coefficient . The potential at short distance does not depend on the energy (rapidity) of the state; it is universal.

In this report, the OPE analysis is applied to QCD, with the aim to theoretically better understand the repulsive core of the NN potential.

2 Operator Product Expansion and potentials at short distance

2.1 General argument

Let us generalize the argument in the introduction, which relates the operator product expansion(OPE) to the short distance behavior of the potential. We write the equal time Bethe-Salpeter (BS) wave function as

(2.0)

where is the eigen-state of the system with the energy , and are some operators of the system. Here we suppress further quantum numbers of the state other than for simplicity. The OPE of and is written as

(2.0)

We here assume that the coefficient function behaves as

(2.0)

if has the same mass dimension of . Therefore the BS wave function becomes

(2.0)

where .

In the approach of Ref.[1, 3, 4], the potential is defined by the BS wave function through the Schrödinger equation as

(2.0)

where is the reduced mass. Since

(2.0)

for the state with angular momentum , the dominant contribution of the potential for non-zero at short distance is trivially given by

(2.0)

As a non-trivial case let us consider the case. There are two cases, depending on the maximum value of defined as .

  1. : In this case, the potential at short distance is universally given by

    (2.0)

    If the interaction is attractive at short distance, while it is repulsive if .

  2. : We denote is the second largest among ’s. The potential at short distance becomes

    (2.0)

    which is attractive for while repulsive for .

2.2 OPE in QCD

Since QCD is an asymptotically free theory, the 1-loop calculation for anomalous dimensions becomes exact at short distance. The OPE in QCD is written as

(2.0)

where () is the renormalized coupling constant (quark mass) at scale . In the limit that ( with fixed ), the renormalization group analysis leads to

(2.0)

where

(2.0)

is the QCD 1-loop beta-function coefficient, and

(2.0)

Here is the 1-loop anomalous dimension of the operator . An appearance of on the right-hand side tells us that it is enough to know the OPE only at tree level. From the above expression, in the previous subsection is given by

(2.0)

Therefore our task is to calculate for 3 and 6–quark operators.

3 Anomalous dimensions for 6–quark operators

3.1 6 quark operators

The OPE of two baryon operators at tree level is given by

(3.0)

where the first term corresponds to the contribution, the second to the , and so on. In this report we consider the case (the first term) only. We denote the general form of a gauge invariant 3–quark operator as

(3.0)

where are spinor, are flavor, are color indices of quark field . The 6–quark operator is constructed from two 3–quark operators as

(3.0)

where and (). Since quarks are fermions, there are some linear dependencies among 6–quark operators. We have to determine a set of independent 6–quark operators. It is not so easy, however, to find them using a quark field basis. Instead we use a simpler method mentioned below.

As the choice of the gauge fixing in perturbation theory, we take the covariant gauge with gauge parameter . Since both the 3–quark operator and 6–quark operator are gauge invariant, must be independent of the gauge parameter . The dependent term in the calculation of at 1-loop becomes

(3.0)

where the -th index of and the -th index of is interchanged in . For example, or . Note that the interchange occurs simultaneously for both and in the above formula. The gauge invariance implies eq.(3.1) , which yields constraints among the 6–quark operators. For example, let us consider the case that and , for which the constraint becomes

(3.0)

where minus signs in the first line come from the property that . There are no further relations among 6–quark operators beyond (3.1).

3.2 1-loop contributions

Only the divergent part of the gauge invariant contribution at 1-loop is necessary to calculate the anomalous dimension of 6–quark operators at 1-loop. The building block of 1-loop calculations is the gluon exchange between two quark lines. If both two quark lines belong to one operator, either or , the contribution is canceled by the renormalization factor of the 3–quark operator , so that the divergent term does not contribute to . If one quark line comes from and the other from , the divergent term contributes to . Suppose that one quark line has indices at one end and at the other end and the other quark line has and . The divergent contribution from the 1-gluon exchange can be expressed as

(3.0)

for or , where and means the right and the left handed component of the spinor indices. Other combinations, or , vanish. This property comes from the fact that the gluon coupling to quarks is chirally symmetric and the chirally non-symmetric quark mass term does not contribute to the divergence.

3.3 Chiral decomposition of 6–quark operators

The physical nucleon operators are constructed from general 3–quark operators as

(3.0)

where is the charge conjugation matrix, are or , and is the Pauli matrix in the flavor space. The spinor index is restricted to the positive energy component such that in the Dirac representation of the matrices.

In this report we consider two nucleon states, which are and . Here we use the notation where is the total spin, is the orbital angular momentum and is the total angular momentum. The 6–quark operator for , which is the spin-singlet and isospin-triplet state, and for (the spin-triplet and isospin-singlet state) are given by

(3.0)

where the summation is taken for the repeated index. Both 6–quark operators have the following chiral decomposition:

(3.0)

where means with and for or .

3.4 Anomalous dimensions

We now give our main results in this report. We define

(3.0)

The eigen-operators of the anomalous dimension matrix are found to correspond to the chirally decomposed operators in the previous subsection. We give the eigenvalue of each operator in table 1, which shows that the operator with zero anomalous dimension always exists and other anomalous dimensions are all negative for both and states. This corresponds to the case (2) of the general discussion in the section 2.1:

  • (, ) for and (, ) for .

The appearance of zero eigenvalues in both and states can be understood as follows. As mentioned in section 3.2, 1-loop contributions to the exist only if spinor indices of two quark lines, one from the other from in , belong to the same chirality (left or right). Since has no such combination, is always zero for this type of operators. As pointed out before, this property is the consequence of the chiral symmetry in QCD interactions.

Table 1: The eigenvalue for anomalous dimension of each eigen operator in and states. In the table means .

4 Conclusion

The OPE and renormalization group analysis in QCD predicts the universal functional form of the nucleon-nucleon potential at short distance:

(4.0)

which is a little weaker than a singularity. We obtain

(4.0)

The anomalous dimension spectrum, however, cannot alone tell whether the potential at short distance is repulsive or attractive. If we evaluate and by the chiral effective theory at the leading order (i.e. the tree level), we obtain

(4.0)

where and is the relative momentum of two nucleons. We find a repulsive core for both states. In particular, in the low energy region such that , the repulsive potential at short distance is almost energy independent, since

(4.0)

Furthermore no low energy constant of the effective theory is required at leading order to obtain the above result.

There are several interesting extensions of the analysis using the OPE. The extension of the OPE analysis to the 3–flavor case may reveal the nature of the repulsive core in the baryon-baryon potentials. Since quark mass can be neglected in this OPE analysis, the calculation can be done in the exact SU(3) symmetric limit. It is also interesting to investigate the existence or the absence of the repulsive core in the 3–body nucleon potential. In this case, we have to calculate anomalous dimensions of 9–quark operators at 2-loop level. More precise evaluations of the matrix element would be preferable. The most straightforward extension is to analyze the tensor force and force by the OPE. Preliminary results indicate that

(4.0)

where force has the strong attractive core at short distance, while no repulsive core exists for the tensor potential. Absence of the repulsive core predicted in the tensor force is consistent with recent numerical simulations[4, 5].

Acknowledgments

S. A. is supported in part by Grant-in-Aid of the Ministry of Education, Sciences and Technology, Sports and Culture (Nos. 20340047, 20105001, 20105003). This investigation was supported in part by the Hungarian National Science Fund OTKA (under T77400).

References

  • [1] N. Ishii, S. Aoki and T. Hatsuda, Phys. Rev. Lett. 99, 02201 (2007).
  • [2] S. Aoki, J. Balog and P. Weisz, Prog. Theor. Phys. 121, 1003 (2009).
  • [3] S. Aoki, T. Hatsuda and N. Ishii, Comput. Sci. Dis. 1, 015009 (2008).
  • [4] S. Aoki, T. Hatsuda and N. Ishii, arXiv:0909.5585 [hep-lat].
  • [5] N. Ishii, S. Aoki and T. Hatsuda, PoS (Lattice 2008), 155 (2008)
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