Valence double parton distributions of the nucleon in a simple model

Valence double parton distribution functions of the nucleon are evaluated in the framework of a simple model, where the conservation of the longitudinal momentum is taken into account. The leading-order DGLAP QCD evolution from the low quark-model scale to higher renormalization scales is carried out via the Mellin moments of the distributions. Results of the valence quark correlation function show that in general the double distributions cannot be approximated as a product of the single-particle distributions.

of the obtained valence dPDF, confirming its crucial effects for the corresponding quark correlation function as the evolution scale is moved up to the experimentally-accessible values. We find that with the increasing renormalization scale, the correlation between the valence quarks becomes large and positive along the edges where x 1 or x 2 is small, while it is negative in the region where x 1 and x 2 are similar and relatively large. This shows in explicit terms that approximating dPDFs with a product of two single-parton distributions (sPDF) is not justified.
Similarly to sPDF, which is interpreted as the probability distribution for the probed parton to carry the fraction x of the total p + momentum of the hadron, the dPDF has the interpretation of the joint probabilistic distribution that the j 1 and j 2 partons carry the momentum fractions x 1 and x 2 of the hadron, respectively. Denoting the sPDF as D j (x) and dPDF as D j 1 j 2 (x ! , x 2 ), one may define the parton correlation function [15; 16] ρ j 1 j 2 (x 1 , As mentioned, a dynamical nonperturbative calculation for the proton has been made in the MIT bag model [15], where the correlations stem from the conservation of the linear momentum (implemented in terms of the Peierls-Yoccoz projection). As is well known, projecting onto good linear momentum coincides with boosting from the rest frame only for the exact eigenstates of relativistic systems [18]. A constituent quark model study has been carried out in [16]. Here we consider a much simpler model which in our view grasps the essential features of the problem and has the proper support. The role of transverse degrees of freedom is discussed at the end.
Let us introduce the probability that the parton carries the momentum fraction x as the square of its wave function, φ (x) = |ψ(x)| 2 . Then the three-particle probability distribution is proposed in the form where the delta function enforces the longitudinal momentum conservation. Its marginal projections define the dPDF and sPDF: Note that Eq. (4) is equivalent to the quark number sum rule of Gaunt and Stirling (GS) [17]. The momentum GS sum rule is also satisfied, as it is straightforward to show that As a matter of fact, the only feature used in these derivations is the symmetric form of Eq. (2). In addition, due to the symmetry, the extremum of D 3 (x 1 , x 2 , x 3 ) is located at the symmetric point x 1 = x 2 = x 3 = 1/3 regardless of its particular shape. Early multiparton models [5] take the simple Regge-motivated parametrization ψ(x) ∼ x a with a = 1 − α(0) and the intercept α(0) = 1/2, while the constant phase-space model of Ref. [19] uses ψ(x) = 1. In this presentation we investigate two simple classes of models of the form where A is a normalization constant such that 1 0 dx φ (x) = 1. We consider the cases α = 0, 1/2, 1 and a = 1, 2. The first class corresponds to the so-called valon model [20; 21] for the proton, which assumes For instance, for the case of the second class with a = 2 in Eq. (6) we get We note that the behavior of D 1 (x) near x → 1 conforms to the QCD counting rules [22]. This is also the case for α = 1 in model I of Eq. (6). As we see, at small x's we can trace a diquark correlation. The above forms hold by construction at the quark-model scale, where the only degrees of freedom are the valence quarks. To relate to results at experimental scales, the appropriate QCD evolution is necessary [23], which generates radiatively the sea quarks and gluons. The matching prescription based on the requirement that at µ = 2 GeV the valence quarks carry the experimental momentum fraction of 41.6% [24] leads to a very low quark model scale, µ 0 = 285 MeV (where the valence quarks carry all the momentum). This low value is compatible to the case of the pion in chiral quark models [25; 26].
The QCD evolution equations for multi-parton distributions have been derived long ago [6; 7]. A simple and practical method of solving them numerically is based on the Mellin moments, similarly to the case of sPDFs. One introduces the corresponding moments of the sPDFs and dPDFs, and the moments of the QCD splitting functions Then the LO dDGLAP evolution equations read [6; 7] d dt M n 1 n 2 where the evolution variable is Partons i, j 1 , and j 2 may in general represent the valence quarks, the sea quarks, or the gluons, whose distributions are coupled. Moreover, the last term in Eq. (10) couples dPDFs to sPDFs. In this talk we consider only the evolution of the valence quarks which leads to a technical simplification, as in this case there are no partons i decaying into a pair of valence quarks and P i→ j 1 j 2 = 0. This means that the inhomogeneous term in Eq. (10) vanishes and our evolution equation simply reads Recall that for sPDFs the corresponding evolution equation is Note that due to the presence of correlations we have M n 1 n 2 j 1 j 2 (t) = M n 1 j 1 (t)M n 2 j 2 (t) and the system is not separable. The solutions of Eq. (12,11) are The inverse Mellin transform brings us to the evolved solution in the x-space, namely where n and n are treated as complex variables and the contours C and C , lying right to all singularities of M, are bended by 45 o (see e.g. Ref. [27]). The bending of the contours helps with the pace of numerical convergence. Schwarz's reflection principle M n * = M * n is satisfied since the anomalous dimensions are real for any integer n and thus one segment of the bended contour is needed in the evaluation. The method is most practical when the moments M are analytic functions of their arguments; if they were not (as could be the case when some numerical fits to the data are made), then they should be approximated with analytic functions, e.g., with sums of the Euler Beta functions, whence the procedure may be carried out with no difficulty.
Next, we proceed to presenting our results of the evolution in the considered model. Before showing the main findings for the valence dPDF, we explore the valence sPDF, where the results can be straightforwardly compared to the existing data parameterizations. Figure 1 presents the valence quark distribution, customarily multiplied by x, evolved to the benchmark scale of µ = 2 GeV and compared to the NNPDF2.3 fits [24], indicated with bands (the darker narrow band is the fit excluding the LHC data, and the broad band uses the collider data only). The reasonable reproduction of the valence sPDF gives us confidence that the simple model of Eq. (3,4)  the evolution on the valence dPDFs is presented in Fig. 2, where we show the contour maps of x 1 x 2 D 2 (x 1 , x 2 ) at three scales: the quark-model scale µ 0 , and the higher scales µ = 2 GeV and µ = 1 TeV. Of course, the support of the function is the region x 1 + x 2 ≤ 1, x i ≥ 0. We observe how the dDGLAP equations cause the drift of the distributions towards low values of x 1 and x 2 . This drift to low values of x is well-known for the case of the DGLAP evolution of sPDFs; it has also been observed for the dPDFs [17]. We note the lack of factorization in the x 1 and x 2 variables within the DGLAP approach, as emphasized in Ref. [28; 29]. The behavior at the end-lines [30] shows that for a fast variable and a slow variable, i.e., x 1 → 1 and x 2 → 0, the correlation becomes small, since a feature confirmed with our numerical analysis. For a probability interpretation to hold, it is necessary that the evolution equations preserve the positivity of the initial condition. Amusingly, it has been found that the upward evolution for sPDFs produces positive distributions [31], unlike the downward evolution where a lower bound for the evolution ratio is found on this basis [27] (cf. also the irreversible evolution of Ref. [32]). Within the considered model, the upward evolution preserves the positivity of the valence dPDF, as can be seen from Fig. 2.
In Fig. 3 we plot the double-parton correlation function as defined in Eq. (1). As the scale increases, the correlation becomes large and positive along the lines x i = 0, while in the central region it is negative. At the line of the kinematic constraint x 1 + x 2 = 1 we find ρ(x 1 , x 2 ) = −1. The results of Fig. 3 show that the valence dPDF cannot be approximated with the uncorrelated product of the sPDFs. We note that our plots bare qualitative similarity to the results obtained in the MIT bag model [15].
We end with some remarks concerning the longitudinal and transverse degrees of freedom. Our calculation is essentially one-dimensional, as the transverse dynamics plays no active role. This dimensional reduction could be possible if the relative momentum between the two quarks is assumed to be small. To analyze this assumption from a non-perturbative point of view, let us remind ourselves that the transverse lattice approach [33] allows to effectively freeze the transverse degrees of freedom when the transverse spacing, a ⊥ , becomes larger than the characteristic resolution of the parton momentum in the hadron, ∼ 1/Λ QCD . This also limits the multiparton Fock state by powers of a ⊥ . For instance, for the nucleon N = q 3 +a 3 ⊥ q 4q +a 4 ⊥ q 3 G+. . .. However, as soon as a ⊥ starts decreasing, gluons and sea quarks are radiated and it is amazing that the DGLAP evolution equations roughly reproduce the observed behavior for sPDF [26].
A simple way to mimic the transverse lattice dynamics is by using a 2-dimensional harmonic oscillator to trap the partons in the hadron [34] in the transverse plane, with a mass squared operator given by Here, x i are the longitudinal momentum fractions fulfilling ∑ i x i = 1, b i are the impact-parameter variables, k ⊥,i their corresponding Fourier-conjugate variables, and σ is the oscillator constant. If ψ n ⊥ (x, b) is the single particle two dimensional HO wave function normalized as d 2 b|ψ n ⊥ (x, b)| 2 = 1 with quantum numbers n ⊥ = (n x , n y ) and mass squared M 2 = 2σ (n x + n y + 1), then the general solution is a symmetrized product of factorized states Due to the fact that the single-particle wave functions have an x-independent normalization, one clearly has Note that here the variables x i are fixed, i.e., they are not dynamical, and we can still multiply by an arbitrary function ϕ(x 1 , . . . , x N ) which would be generated after requantization by some unspecified 1-dimensional dynamics, say M 2 = M 2 HO + M 2 1+1 . Our model in Eq. (2) corresponds to the product ϕ(x 1 , . . . x N ) = ∏ i ψ(x i ). This is similar to the Born-Oppenheimer approximation where the longitudinal variables obbey classical dynamics. In this extreme case the mass terms give after minimization x i = m i /m, with m = ∑ i m i yielding a contribution m 2 to M 2 and D N (x 1 , . . . , x N ) → ∏ i δ (x i − m i /m), which for equal masses corresponds to locating the distridution in our Eq. (2) at the maximum, x i = 1/N. That model breaks the transverse translational invariance, which can be restored by projecting onto zero total transverse momentum using the Peierls-Yoccoz method [18], such that for m i = 0 one finds M 2 N = 2Nσ for the symmetric state. A straightforward calculation with the rest frame wave function yields the following result for the unintegrated dPDF: Thus, there exists a transverse dynamics given by Eq. (18) where the effective 1-dimensional treatment used here holds, but it does not support the often assumed transverse-longitudinal factorization.