UNIFIED DISPERSIVE APPROACH TO \gamma^{*}\to\gamma\pi\pi AND \gamma\gamma\to\pi\pi

# Unified Dispersive Approach to γ∗→γππ and γγ→ππ

B. Moussallam
###### Abstract

A representation of the amplitude is proposed which combines large chiral resonance Lagrangian modelling with general unitarity and analyticity properties. The amplitude is constrained from scattering results and measurements by the CMD-2 and SND collaborations. As an application, the contribution of the states in the HVP contribution to the muon are reconsidered, taking into account the effect of the strong -wave rescattering in a model independent way.

Received Day Month Year

Revised Day Month Year

## 1 Introduction

The leading hadronic contribution to the muon is associated with the hadronic vacuum polarization (HVP) function, and the contribution from , proportional to the square of the pion form factor, dominates the HVP unitarity relation. This has triggered experimental efforts for measuring the pion form factor to high accuracy, in particular, via the initial-state radiation (ISR) method (see  and references therein). In the cross-section, the final-state radiation (FSR) amplitude contributes in addition to the ISR. In principle, they could be separated experimentally by performing a partial-wave analysis. The FSR amplitude is also needed for computing the contribution in the HVP unitarity relation. In practice, the FSR amplitude is often estimated using the sQED approximation, which treats the pions as point-like and non-interacting. It ignores, in particular, the influence of the strong -wave attraction at low energy. A modelling of this effect using a narrow -meson gives surprisingly large results . We discuss here an approach in which rescattering is treated in the model independent Omnès method . It can be viewed as a generalization of classic work on the amplitude  and uses scattering experimental results as constraints. A further generalization to the case of two virtual photons is presented at this conference , which will be applied to the light-by-light hadronic contribution to the .

## 2 Analyticity of partial-waves when q2≠0

The Omnès method applies to partial-wave projected amplitudes, it combines the unitarity relation and analyticity properties. We restrict ourselves here to the elastic scattering region GeV which will limit the applicability of the amplitude to virtualities GeV. In the case of two real photons, the partial-wave amplitude is an analytic function of the energy , except for two cuts, the right-hand cut which lies on and the left-hand cut on . The discontinuity across the right-hand cut is given by the unitarity relations, these have exactly the same form for and amplitudes. In contrast, the left-hand cuts differ. The main issue is to properly define this cut and verify that no anomalous threshold is present.

The left-hand cut is associated with singularities of the unprojected amplitude in the crossed channels. One firstly has the pion pole in the amplitude (so-called Born amplitude) the projection reads,

 hBorn0,++(s,q2)=Fvπ(q2)s−q2[4m2πσπ(s)Lπ(s)−2q2],  Lπ(s)=log1+σπ(s)1−σπ(s) (1)

with . Having affects the amplitude through the pion form factor but also the singularities: the Born amplitude displays a pole at in addition to a left-hand cut. Using the prescription moves the pole away from the right-hand cut when . Secondly, one must consider the cuts associated with . These processes are expected to display sharp resonance effects below 1 GeV from the vector mesons , . We may start with a large approximation, where resonances generate simple poles in (note that scalar mesons, which violate large rules are not allowed). Using a resonance chiral Lagrangian, the contributions from a vector meson exchange to the three independent invariant amplitudes read

 AV(s,t,q2)=~CVFVπ(q2)[s−4m2π−4t+q2t−M2V+s−4m2π−4u+q2u−M2V]BV(s,t,q2)=~CVFVπ(q2)[12(t−M2V)+12(u−M2V)]CV(s,t,q2)=~CVFVπ(q2)[1t−M2V−1u−M2V] (2)

The main difference when is from the kinematics: for the Mandelstam variables , are negative while for they lie in the range: . One must then take the width of the resonance into account, and this must be done in a way consistent with the general analyticity properties for, otherwise, the Omnès method would not be applicable. This may be implemented by using a Källén-Lehmann representation, i.e. by replacing, in eq. (2)

 1M2V−w⟶˜BWV(w)=1π∫∞4m2πdt′σ(t′,MV,ΓV)t′−w,w=t,u (3)

The function has a cut on the first Riemann sheet, while a pole appears on the second sheet. The cut structure of the partial-wave projection of the vector-exchange amplitude is illustrated on figs. 1: the left figure shows that the cut extends into the complex plane and approaches the right-hand cut. The vicinity of the right-hand cut is illustrated on the right figure. Thanks to the analytic propagator and the prescription, no intersection actually occurs, which guarantees the absence of an anomalous threshold and the applicability of the usual Omnès method.

## 3 Soft photon, chiral and experimental constraints

We consider an Omnès representation for the amplitudes based on twice-subtracted dispersion relations i.e. involving two polynomial parameters for each isospin . These account e.g. for higher mass resonances not explicitly included and depend on . Beside the properties of analyticity and elastic unitarity, there are additional physical constraints that must be imposed. Gauge invariance imposes that the amplitudes minus the Born term must vanish in the soft photon limit  which eliminates one of the parameters for each . The helicity amplitude , where is the cosine of the scattering angle in the CMS, can be written as

 HI++(s,q2,z)=HI,Born++(s,q2,z)+∑V=ρ,ωHI,V++(s,q2,z)+HI,resc++(s,q2,z) (4)

The last term in eq. (3) accounts for the rescattering in the partial-wave, it reads

 HI,resc++(s,q2,z)=ΩI0(s){(s−q2)bI(q2)+sFvπ(q2)[s(JI,π(s,q2)−JI,π(q2,q2))s−q2HI,resc++()−q2^JI,π(q2)]+s∑V=ρ,ωFVπ(q2)[sJI,V(s,q2)−q2JI,V(q2,q2)]} . (5)

is the usual Omnès function and , are the related integrals (see ) involving the partial-wave projections of the Born and the vector-exchange amplitudes respectively. Finally, at . The other helicity amplitudes , are affected by rescattering from partial-waves.

The two functions , , are constrained by chiral symmetry. In the exact chiral limit, the amplitude for producing a pair satisfies a soft pion theorem: it vanishes at for any value of . In the real world, the Adler zero moves to and depends on . The correct chiral behaviour is enforced by matching the dispersive amplitudes for both and with the corresponding chiral expansion expressions  at and small . For larger values of GeV the dependence is dominated by the light vector resonances. Introducing the combinations and corresponding to the and channels, the following parametrization encodes these properties

 bn(q2)=bn(0)Fχ(q2)+FR(q2),bc(q2)=bc(0)+FR(q2) (6)

where involves the Gounaris-Sakurai and Breit-Wigner functions, and . The values of , are determined from the polarizabilities of the and the which we take to be compatible with the chiral predictions. In the parametrization (3) we used the same resonance function for and i.e. we neglected the resonance contribution to . This is justified from the fact that the Omnès functions satisfy the inequality in the physically relevant region which suppresses the influence of . Thanks to this simplification, determining the two parameters , from allows one to predict . A combined fit to the two data sets from the SND and CMD-2 collaborations  gives: , GeV with , this is illustrated in Fig.2.

## 4 Application to the ππγ contributions to the muon g−2

The contribution of the HVP to the muon which involve two pions plus one photon can be written in terms of infrared finite cross-sections,

 g−22∣∣∣ππγ=14π2∫∞4m2πdq2Kμ(q2)(σsQEDe+e−→π+π−γ(q2)+∑n,c^σn,ce+e−→ππγ(q2)) (7)

where (see e.g.  for the explicit expression of the functions and )

 σsQEDe+e−→π+π−γ=α33q2σ3π(q2)|Fvπ(q2)|2×η(q2)^σc,ne+e−→ππγ=α312(q2)3∫q24m2πds(q2−s)σπ(s)∫1−1dz(|^Hc,n++|2+|^Hc,n+−|2+|^Hc,n+0|2) (8)

where and .

The contributions to the muon , restricting the integration range in eq. (4) to GeV, within the domain of validity of the model, are shown in table 1. As compared to previous work, we find for the contribution linear in a different sign than ref. , which is due to the effect of the rescattering. The results from the last two lines can be compared with ref.  who use a sigma resonance approximation: our result is smaller in magnitude by a factor of three. The table shows that the sQED contribution is largely dominant. Still, it would be of interest to be able to extend the integration range somewhat since one expects a kinematical increase of when . This would necessitate to include rescattering, which is easy to implement, and also account for inelasticity.

Acknowledgements: Supported by the European Community-Research Infrastructure Integrating Activity ”Study of Strongly Integrating Matter” (acronym HadronPhysics3)

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