<svg xmlns:xlink="http://www.w3.org/1999/xlink" xmlns="http://www.w3.org/2000/svg" style="vertical-align:-4.17203pt" id="M1" height="12.0921pt" version="1.1" viewBox="-0.0657574 -7.92007 21.6701 12.0921" width="21.6701pt"><g transform="matrix(.017,0,0,-0.017,0,0)"><path id="g50-238" d="M583 449L551 460C535 436 529 433 494 433C409 433 311 438 228 438C97 438 53 381 24 341L44 316C85 355 124 372 183 372C161 259 87 53 26 5L34 -12C53 -12 94 -4 118 12C166 92 211 256 236 371L394 369C375 301 352 212 334 121C329 96 326 75 326 58C326 5 349 -12 381 -12C431 -12 482 25 519 66L504 97C480 80 448 64 432 64C419 64 410 80 422 154C432 217 450 303 466 365C499 365 536 366 546 369C557 384 570 409 583 449Z"/></g><g transform="matrix(.012,0,0,-0.012,9.884,3.961)"><path id="g50-102" d="M398 365C398 411 356 451 297 451C250 451 198 430 151 397C65 336 24 230 24 139C24 14 97 -12 148 -12C198 -12 284 7 373 104L355 130C306 84 246 53 198 53C132 53 111 109 111 163V189C209 211 398 261 398 365ZM317 351C317 308 273 262 117 225C134 338 189 383 221 399C230 404 249 407 263 407C295 407 317 389 317 351Z"/></g><g transform="matrix(.012,0,0,-0.012,14.953,3.961)"><path id="g50-52" d="M290 377C321 398 342 415 358 430C378 450 389 473 389 502C389 578 329 635 238 635H237C184 635 137 610 109 578L64 515L88 493C112 529 154 573 208 573S303 542 303 482C303 409 233 370 141 341L149 308C165 313 190 319 215 319C272 319 341 283 341 193C342 98 292 43 222 43C163 43 122 72 96 94C88 101 79 100 70 94C61 87 47 73 46 60C44 47 48 37 62 23C76 10 118 -12 165 -12C238 -12 430 62 430 223C430 297 379 359 290 375V377Z"/></g></svg> Form Factor <svg xmlns:xlink="http://www.w3.org/1999/xlink" xmlns="http://www.w3.org/2000/svg" style="vertical-align:-4.4924pt" id="M2" height="16.753pt" version="1.1" viewBox="-0.0657574 -12.2606 17.0953 16.753" width="17.0953pt"><g transform="matrix(.017,0,0,-0.017,0,0)"><path id="g50-103" d="M620 667C620 684 593 710 552 710C515 710 459 687 409 634C360 582 334 506 320 433H247L215 400L220 388H310L259 80C224 -129 199 -161 185 -174C175 -183 160 -192 141 -192C123 -192 90 -181 75 -165C69 -158 64 -156 54 -164C39 -178 24 -195 24 -208C24 -231 61 -257 94 -257C124 -257 162 -243 209 -194C267 -134 303 -66 343 107C369 220 378 279 393 385L503 397L523 433H404C432 619 464 660 500 660C522 660 542 646 566 621C573 614 583 615 593 621C603 628 620 648 620 667Z"/></g><g transform="matrix(.012,0,0,-0.012,8.906,3.961)"><path id="g54-33" d="M556 236V289H56V236H556Z"/></g></svg> Near the Mass Shell

Krivoruchenko, M. I.

doi:https://doi.org/10.1155/2015/656239

Advances in High Energy Physics

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Abstract Introduction Acknowledgments References Copyright Related Articles

Research Article | Open Access

Volume 2015 | Article ID 656239 | https://doi.org/10.1155/2015/656239

Form Factor Near the Mass Shell

M. I. Krivoruchenko^1,2,3

Academic Editor: Enrico Lunghi

Received29 Nov 2014

Accepted06 Apr 2015

Published27 May 2015

Abstract

The generalized Ward-Takahashi identity (gWTI) in the pion sector for broken isotopic symmetry is derived and used for the model-independent calculation of the longitudinal form factor of the vector vertex. The on-shell is found to be proportional to the mass difference of the pions and the difference between the vector isospin and scalar isospin pion radii. A numerical estimate of the form factor yields a value two times higher than the previous estimate from the quark model. Off-shell form factors are known to be ambiguous because of the gauge dependence and the freedom in the parameterization of the fields. The near-mass-shell appears to be an exception, allowing for experimental verification of the consequences of the gWTI. We calculate the near-mass-shell using the gWTI and dispersion techniques. The results are discussed in the context of the conservation of vector current (CVC) hypothesis.

1. Introduction

The decay () is one of the main semileptonic electroweak processes. The vector nature of the transition, its simple kinematics, and the precise measurement of the partial width make this decay particularly attractive for testing the Standard Model.

The decay amplitude is proportional to the element of the Cabibbo-Kobayashi-Maskawa (CKM) matrix. Radiative corrections and pion structure effects in the decay have been calculated with high accuracy [1–6], sufficient for verification of the unitarity of the CKM matrix. The experimental data, however, are not yet sufficiently precise for this purpose [7, 8].

Measurements of the decay are also motivated by the possibility of testing the conservation of vector current (CVC) in the meson sector. The CVC hypothesis [9–11] suggests that the isovector component of the electromagnetic current and the charged components of the weak vector current belong to the same isospin triplet. In the limit of exact isotopic symmetry, conservation of the electromagnetic current implies conservation of the weak vector current.

Off the mass shell, the CVC is equivalent to the Ward-Takahashi identity (WTI) for the isospin group. The WTI, however, is of greater generality and leads to useful relationships between off-shell form factors, including those that vanish when some of the external legs are on shell. The violation of isotopic symmetry, associated with the small mass difference between the up and down quarks and the electromagnetic and weak interactions, results in the nonconservation of the charge-changing components of the weak vector current. For the broken symmetry, the CVC condition and the WTI are replaced by partial CVC and the generalized WTI (gWTI), which are especially sensitive to the pattern of isotopic symmetry breaking.

Off-shell form factors enter the descriptions of nucleon knockout reactions [12, 13] and bremsstrahlung reactions [14]. As a result of shifting away from the mass shell, the electromagnetic currents of bound nucleons are different from the free currents, which also leads to observable effects [15].

The parameterization of the degrees of freedom associated with the pion field can be performed in various ways, which produces off-shell ambiguity in the amplitudes. The on-shell form factors are related to the asymptotic states and are uniquely defined. This statement is known as the equivalence theorem (ET) [16–18]. The off-shell form factors, although they contribute to the physical amplitudes, depend on this parameterization and cannot be measured experimentally [19, 20].

We report a notable exception to this rule. The longitudinal part of the vertex is shown to be uniquely defined near the mass shell and fundamentally accessible to measurements, and therefore, it can be investigated for its consistency with the gWTI.

In quark models, pions are usually poorly described because of their Goldstone boson nature. As an application of the gWTI, we derive a model-independent expression and provide a numerical estimate for the longitudinal form factor . The structure of this paper is as follows. Section 2 begins with a discussion of the constraints imposed by the WTI of the symmetry group on the electromagnetic pion form factors. In Section 3, a generalization of the WTI for broken isotopic symmetry is derived, and in Section 4, it is used to find the relationships between weak vector form factors. The near-mass-shell form factor is then expressed in terms of the pion mass difference and the pion radii in the isospin and channels. In Section 5, we focus on extracting the isospin pion radius from the experimental data on -scattering phase shifts and numerically evaluate . Finally, we conclude in Section 6 with a summary and a discussion.

2. Vector Vertex

The on-shell conserved vector current of a charged scalar particle is determined by one form factor. Off the mass shell, there are two form factors. In the most general case, the current can be written as follows:where is the momentum transfer. The form factors are symmetric functions of and and arbitrary functions of and the physical mass of the charged pion. The factor in the second term is added to ensure the negative parity of the current. The form factor decomposition (1) arises in scalar quantum electrodynamics (QED) (see, e.g., [21]) and in chiral perturbation theory (PT) (see, e.g., [22]). The WTI of the symmetry group establishes a relationship between and that is identical to that of (4).

Isotopic symmetry implies that the mass difference of nonstrange quarks can be neglected and that the electromagnetic and weak interactions are switched off beyond tree level. In this limit, the weak interaction is described by an isovector current , where the are isospin generators. As a result, exact CVC occurs: a dressed vertex forms an isospin triplet, and the weak vector current is conserved.

The WTI associated with the symmetry group imposes a constraint on the vertex (see, e.g., [23]):where is the renormalized pion propagator. The self-energy operator satisfiesCombining (2) with (1) yieldsIn the limit , we obtainIn the vicinity of , the form factor can be expanded to givewhere is the vector charge radius.

The pion form factor , which describes strong interaction effects, is an analytic function of the complex variable at least in the circle . The nearest to the mass shell singularity at is caused by the three-pion threshold. A Taylor series in powers of converges within that circle. The same is true for the variable . A Taylor series in powers of converges for , where the radius of convergence is determined by the two-pion threshold.

The equivalence of the Coulomb and Lorentz gauges in QED was rigorously proved in [24, 25]. On shell, the amplitudes are gauge invariant, whereas the off-shell dependence on the gauge persists. and, by virtue of (5), are thus uniquely defined, when both legs of the charged pion are on the mass shell. To first order in the displacement from the mass shell, the longitudinal component of the vertex is also gauge invariant, as is evident from (1). Aside from these cases, depends on the gauge and cannot be measured.

with two on-shell legs does not contribute to the current. Off the mass shell, however, does contribute, and its contribution is uniquely determined by the WTI. Isotopic rotation of is not sufficient to obtain a full weak-interaction vertex. We show that the violation of isotopic symmetry generates an isospin contribution that is unrelated to isotopic rotation.

3. Generalized Ward-Takahashi Identity for Broken Isotopic Symmetry

In order to find the longitudinal form factor of the weak vector current, we derive a generalization of the WTI that is associated with the replacement of the exact symmetry by the broken symmetry.

Let us consider the variation of the pion propagatorunder the transformationIn terms of a Cartesian basis, the pion field is Hermitian, and is an infinitesimal imaginary antisymmetric matrix that can be expanded in the group generators with real coefficients . In the conventional normalization, . The variation of the pion propagator is given byIn matrix notation, .

Independent calculation of involves the effective Lagrangian, which we consider to be of the formwhere , is the electromagnetic field, , and is the weak vector field associated with and bosons. In a Cartesian basis, is real. The isotopic invariance in is broken by the mass term with and by the electromagnetic and weak interactions. In other respects, is an arbitrary function, which reflects the ambiguity in the parameterization of the pion field.

The combination of ensures the implementation of the CVC condition at a bare interaction vertex: the electromagnetic current coincides with the third component of the weak vector current by construction. If the isotopic symmetry in would not have been broken, the CVC condition could also hold for a dressed vertex, and the weak vector current could also be conserved. In the case of this broken symmetry, however, the dressed vertex acquires an admixture of tensor components, while the charge-changing weak vector current is no longer conserved. The WTI can be viewed as a generalization of the CVC for an off-shell vertex. It permits generalizations for broken symmetries; thus, when the isotopic symmetry is broken, the CVC becomes partial CVC, whereas the WTI of the exact isotopic symmetry turns into the WTI of the broken isotopic symmetry.

Transformation (8) is equivalent to the compensating transformation in :which generates variations of the pion mass term and the vector fields in :As a result, acquires the correctionwhereare the vector and scalar currents of the pion.

The response of the pion propagator to the compensating transformation iswith vertex functions defined byNow, let us consider momentum space:Combining (9) and (15) leads toThis equation generalizes the WTI for the broken symmetry. It is shown graphically in Figure 1.

4. Vector Vertex

In a Cartesian basis, , which means that . Given that , the pion propagator is symmetric under transposition of the isospin indices: .

The isospin content of a matrix can be determined using projection operators:Among symmetric matrices, there are only isospin-0 or isospin-2 matrices that are proportional to the unit matrix or to quadratic forms of . The allowed pion mass operator is therefore , where the are numbers. The charged pions are degenerate in mass; therefore, invariance holds.

The vertex functions obeyThe functions and depend on the variables , and . Symmetry (antisymmetry) in the isospin indices implies that vertex function is symmetric (antisymmetric) under the permutation of and . Functions that are symmetric in isospin describe states with isospin and , whereas those that are antisymmetric describe isospin states. Similar properties characterize the form factors of .

The vertex functions can be expanded in scalar functions that are symmetric in and . The lower index indicates the symmetry with respect to permutation of the isospin indices: (). The expansion takes the form

If there was no isospin symmetry breaking, we could have , as there are no other generators, and , implying that and .

The gWTI (18) can be split into isospin-symmetric and isospin-antisymmetric parts:where is a commutator and is an anticommutator.

Consider some of the consequences of (23). For , , we obtainIn a cyclic basis, the generators are equal to and . The left-hand side of (25), when sandwiched between the initial and final states in the pion decay, gives the pion mass difference:where and . In the more general case of and , one findsThe trace of the commutator of finite-dimensional matrices vanishes, and therefore, the left-hand side of (25) and (27) describes a state of total isospin 2. The isospin-zero component of (27) satisfies the equation . At zero momentum transfer, , and the overall normalization of the form factors is not fixed. In the channel of the pion decay, the state has the isospin projection, so the channel is of no interest.

As a consequence of elastic unitarity and analyticity, the dependence of the on-mass-shell form factor is determined by the Jost function that can be constructed in terms of the phase shift in the corresponding channel (see, e.g., [23]). We consider an -wave because the last three vertices in induced by the transformation (11) do not contain derivatives of , and thus, the -wave channel of the pion-pion scattering is relevant. We therefore writewhere . The value of is proportional to the mass splitting in the pion multiplet. We restrict ourselves to the first order in . Accordingly, the physical pion masses in the arguments of the vertex functions can be replaced by a mean value, for example, , provided that these functions, such as and , are already small. Using (25)–(28), we obtain where

Let us consider the consequences of (24). Equation (21) shows that can be evaluated with the required accuracy in the limit of exact isotopic symmetry with and . On the mass shell, moreover, , and thus,To the leading order of the expansion in , the form factor is determined by the isotopic rotation of the electromagnetic form factor (5).

The form factors , as defined by (30) and (31), are not singular at . For small , they are determined by the pion radii. The on-shell weak vector current is usually parameterized in the formwhere .

The exact CVC condition implies

Partial CVC, as follows from the comparison of (21) and (32), yieldsThe isovector part is recovered from the electromagnetic vertex, whereas the isotensor part is independent of it. Remarkably, for a dressed vertex, the boson, being a member of the weak isospin triplet, is coupled to both the strong isospin triplet and the strong isospin quintet.

Equation (34) can also be derived in a simpler and more direct way, analogously to the standard analysis of decays [26].

First, we introduce the form factorswith . In the channel, the space-like component of the current is proportional to , whereas the time-like component is proportional to . By applying the -channel unitarity condition for the form factors, we find that is determined by the scattering amplitude, whereas is determined by the scattering amplitude, where is the angular momentum of the pions. and can thus be identified as vector and scalar form factors, respectively, which is consistent with the gWTI.

Second, we assume an expansion in for both and . This assumption conveys the analyticity of the form factors. Equation (36) leads tosuch that we recover (34) and, in addition, observe that it is exact for the on-shell case. However, the connection to the CVC condition remains hidden in this simplified approach.

The nature of the form factor can also be clarified with the aid of (32). Taking the scalar product of both sides of the equation with the vector yieldsOn the left-hand side, we obtain the form factor, which is a Lorentz scalar. Equation (38) is the formal statement of the nonconservation of the lowering component of the weak vector current.

Equation (34) can therefore be derived using either the gWTI or the kinematic decomposition of (35) and (36). Because recourse to the gWTI is optional, (34) is less interesting for testing the gWTI. We therefore analyze the form factors off the mass shell.

The WTI of exact symmetry implies, to first order in the displacement and for low momentum transfers,

The WTI of broken symmetry implies, to first order in and the displacement and for low momentum transfers,

The decay rate depends on the near-mass-shell behavior of the form factor . Any such reaction may serve for testing the gWTI.

For large momentum transfers, the pion radii in (34), (39), and (40) should be replaced with the form factors of (30) and (31). Expressions (33), (34), (39), and (40) correspond to the various versions of the CVC condition.

The on-shell form factor is independent of both the gauge and the parameterization. By virtue of (30) and (31), the on-shell form factors are also uniquely defined. The longitudinal component of the vertex (21) contains the factor in , whereas has smallness of . We thus conclude that the longitudinal component of is uniquely defined in the neighborhood of the mass shell to first order in the pion mass splitting and the displacement . In the neighborhood of the mass shell, the form factor thus avoids the general rule [16–20, 24, 25] that states that off-shell amplitudes are ambiguous.

The results obtained for the near-mass-shell representation of in terms of the physical masses and radii of the pions exhibit explicit independence of the gauge and the parameterization of the pion field.

From a mathematical point of view, one can speak of the uniqueness of the longitudinal component of in an infinitesimal neighborhood of the mass shell or, equivalently, of the uniqueness of the longitudinal component of and its first derivatives with respect to and on the mass shell to first order in the pion mass splitting.

The transverse component of the vertex does not exhibit any specific behavior, and thus, we consider to be ambiguous off shell.

The generality of the relationships (34) and (40) is influenced by only the CVC condition at a bare interaction vertex. This condition is satisfied in the Standard Model, so any violation of these relationships can be interpreted as an indication for new physics at or above the electroweak scale.

5. Numerical Estimates

In this section, we employ the dispersion techniques for numerical estimation of the pion radius , entering (34) and (40), and of the form factor .

In the scattering of pions, the inelastic channels do not become relevant until an invariant mass of 1.2 GeV [27–29]. The elastic scattering amplitude is determined by the phase shift through the Jost function:The unitarity relation for the form factor implies (cf. (28))where is a finite-degree polynomial. The degree of can be fixed by the quark-counting rules, which, in our case, take the form for . The asymptotes of the Jost function are determined by value of the phase at infinity. The experimental phase is known for energies up to GeV. At this energy, . If one takes for GeV, then the quark-counting rules are not satisfied, even for the zero-degree polynomial . The minimal required modification is to introduce a hypothetical resonance with mass . Such a resonance should have a large width because it is not observed experimentally. Note that, in the Veneziano model, there are no resonances in the channel. The contribution of a large is suppressed in the dispersion integral by the inverse of the second power of , and one can assume that this contribution is not dominant. The contribution of the large- region can be evaluated by comparing the contributions of the intervals GeV and GeV, for which experimental data are available. A polynomial of degree requires resonances. If there are primitives, then the number of resonances increases. The numbers of resonances and primitives are correlated with the number of Castillejo-Dalitz-Dyson poles [30].

Expanding the Jost function in the vicinity of , we obtainFor numerical estimates, the upper limit of the integral is replaced by ; the scattering phase shift between the experimental points is interpolated linearly. The results are shown in Table 1 for the data sets from [27–29]. A further refinement of the estimate can be done using more theoretical inputs from semiphenomenological models of pion-pion scattering [31] and lattice QCD [32].

The negative “mean square radius” occurs because of the negative -channel scattering phase, which is a signature of repulsion. In the general case, the mean square radius is defined as the first expansion coefficient of the corresponding form factor in powers of , and the sign of this expansion coefficient is not fixed a priori. Vector boson exchange produces repulsive forces between identical particles. The channel with contains a pair of positively charged pions, and thus, the repulsive nature of the phase can be attributed to the dominance of the -channel -meson exchange between the pions.

Equation (43) has a variety of applications. In the zero-width approximation with , where is the mass of the meson, one arrives at the well-known expression for the pion charge radius, . In the channel with an attraction, becomes positive and approaches the experimental value, thereby supporting the vector meson dominance model. The pion scalar radius can be determined using the data for pion-pion scattering in the channel, yielding [33]. The positive value of reflects the dominance of the attractive interaction, which is consistent with the existence of the meson.

In the dispersion theory, the contribution from the high energy part of the dispersion integrals is considered to be the important source of theoretical uncertainties. The representation (41) is justified in an approximation of neglecting all the inelastic channels. In our case, the elasticity holds for GeV [27–29], so the dispersion integral from this region accurately assesses the contribution to the pion radius. With increasing the energy above 1.2 GeV, the parameter of inelasticity increases smoothly up to 0.5 for GeV. The part of the integral (43) corresponding to this region gives therefore an approximate estimate of the contribution. Using results of [28], we find that this contribution is numerically small and equals only . The uncertainty associated with higher energies GeV can be estimated by assuming the existence of a hypothetical resonance with mass GeV. In the zero-width approximation, the error equals for GeV, which is comparable to the experimental uncertainty of the contribution from the interval GeV.

Experimental value of the charge radius equals [34]. Using the value , we obtain with the help of (34) which is a factor of two greater than the light-front quark model prediction [5]. The estimated error corresponds to the experimental errors in the -scattering phases and the uncertainty of the high energy part of the integral representation (43).

Contribution of the longitudinal form factor to the decay rate can be estimated to give ; the additional small factor in arises for kinematic reasons. The experimental error in is 0.6% [34]. We thus reaffirm earlier conclusions that is currently beyond the capabilities of the experimental study. The possibility of measuring the longitudinal weak vector current in the neutron decay [35], muon capture [36], and in the and decays is, perhaps, more promising.

A favorable experimental situation exists in the decays. The large difference in the masses of - and -mesons hampers the near-mass-shell expansion, so the decays seem to be not suitable for the measuring off shell and testing the gWTI. At the same time the dispersion techniques allowing determining on shell have found in these decays a successful application [37, 38].

The dominant part of is electromagnetic in origin [39–41]. Small mass difference between up and down quarks leads to the mixing, which also contributes to . Equation (34) describes therefore the electromagnetic contribution of order to the longitudinal weak vector current and the small mixing effect.

PT has been very successful in describing properties of light mesons in the nonperturbative regime [40–43]. Predictions for the -scattering lengths, first obtained by Weinberg [44] and improved by the development of PT, agree with experiment to a high degree of accuracy [45, 46]. The pion radii and are also well understood [33, 40, 47, 48], while the pion radius has not been discussed so far. The embedding of isotopic symmetry breaking into the PT framework on line with [3, 4, 41, 49] could allow also describing the near-mass-shell form factor , starting from the first principles of QCD.

6. Conclusion

In this paper, the longitudinal component of the weak vector current in the decay was calculated. This component arises due to the violation of isotopic symmetry by the pion masses and the electromagnetic and weak interactions. A generalization of the WTI was derived in the pion sector to account for the isotopic symmetry breaking. It was shown that the isovector part of the current can be reconstructed through isotopic rotation of the off-shell pion electromagnetic form factors, whereas the isotensor part has no analogs but rather is uniquely determined by the gWTI combined with the elastic unitarity, analyticity, and the pion-pion scattering data. Because of the low momentum transfer, the on-shell form factor is proportional to the pion mass difference and the difference of the vector-isovector and scalar-isotensor pion radii. The relationship between the near-mass-shell form factor and the pion radii (40) is a consequence of the CVC condition extended beyond the approximation of exact isotopic symmetry.

The various versions of the CVC condition are distinguished depending on whether the isotopic symmetry is exact or broken and whether the outer legs in the vertex are on or off shell. The corresponding predictions for the longitudinal form factor are given in (33), (34), (39), and (40). In the case of the exact isotopic symmetry, the bare and dressed weak vertices are pure isospin triplets; the CVC and the WTI hold on and off shell, respectively. In the case of the broken isotopic symmetry, the dressed weak vertex is no longer a pure isospin triplet; partial CVC and the gWTI hold on and off shell.

Favorable conditions for testing the gWTI by measuring the longitudinal weak vector current appear to exist in the and decays with soft photon emission because of the involvement of the near-mass-shell form factors, the relatively large momentum transfer in the weak vertex, and the small mass differences within the pion and kaon multiplets.

A nontrivial consequence of partial CVC occurs in the off-shell case, in which the vertex in general is not gauge invariant and depends on the parameterization of the pion field. The only exception is the longitudinal component of the vertex in the neighborhood of the mass shell. To first order in the pion mass splitting and the displacement from the mass shell, the longitudinal component is independent of both the gauge and the parameterization, and therefore, the near-mass-shell form factor appears to be a unique object whose properties are unambiguously determined by the partial CVC condition (the gWTI) and also fundamentally allow for experimental verification.

Conflict of Interests

The author declares that there is no conflict of interests regarding the publication of this paper.

Acknowledgments

This work was supported by RFBR Grant no. 13-02-01442, Grant no. HLP-2015-18 of Heisenberg-Landau Program, and Grant no. 3172.2012.2 for Leading Scientific Schools of Russian Federation.

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Copyright © 2015 M. I. Krivoruchenko. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited. The publication of this article was funded by SCOAP³.

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