Neutrino Physics in the Frontiers of Intensities and Very High Sensitivities 2016
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P. Sarriguren, O. Moreno, E. Moya de Guerra, "Nuclear Structure Calculations for TwoNeutrino Doubleβ Decay", Advances in High Energy Physics, vol. 2016, Article ID 6391052, 12 pages, 2016. https://doi.org/10.1155/2016/6391052
Nuclear Structure Calculations for TwoNeutrino Doubleβ Decay
Abstract
We study the twoneutrino double decay in ^{76}Ge, ^{116}Cd, ^{128}Te, ^{130}Te, and ^{150}Nd, as well as the two GamowTeller branches that connect the double decay partners with the states in the intermediate nuclei. We use a theoretical microscopic approach based on a deformed selfconsistent mean field with Skyrme interactions including pairing and spinisospin residual forces, which are treated in a protonneutron quasiparticle randomphase approximation. We compare our results for GamowTeller strength distributions with experimental information obtained from chargeexchange reactions. We also compare our results for the twoneutrino double decay nuclear matrix elements with those extracted from the measured halflives. Both singlestate and lowlyingstate dominance hypotheses are analyzed theoretically and experimentally making use of recent data from chargeexchange reactions and decay of the intermediate nuclei.
1. Introduction
Double decay is currently one of the most studied processes both theoretically and experimentally [1–5]. It is a rare weakinteraction process of second order taking place in cases where single decay is energetically forbidden or strongly suppressed. It has a deep impact in neutrino physics because the neutrino properties are directly involved in the neutrinoless mode of the decay () [6–8]. This decay mode, not yet observed, violates leptonnumber conservation and its existence would be an evidence of the Majorana nature of the neutrino, providing a measurement of its absolute mass scale. Obviously, to extract a reliable estimate of the neutrino mass, the nuclear structure component of the process must be determined accurately. On the other hand, the double decay with emission of two neutrinos () is perfectly allowed by the Standard Model and it has been observed experimentally in several nuclei with typical halflives of years (see [9] for a review). Thus, to test the reliability of the nuclear structure calculations involved in the process, one checks first the ability of the nuclear models to reproduce the experimental information available about the measured halflives for the process. Although the nuclear matrix elements (NMEs) involved in both processes are not the same, they exhibit some similarities. In particular, the two processes connect the same initial and final nuclear ground states and share common intermediate states. Therefore, reproducing the NMEs is a requirement for any nuclear structure model aiming to describe the neutrinoless mode.
Different theoretical approaches have been used in the past to study the NMEs. Most of them belong to the categories of the interacting shell model [10–12], protonneutron quasiparticle randomphase approximation (QRPA) [1, 2, 13–25], projected HartreeFockBogoliubov [26–28], and interacting boson model [29–31].
In this work we focus on the QRPA type of calculations. Most of these calculations were based originally on a spherical formalism, but the fact that some of the double decay nuclei are deformed makes it compulsory to deal with deformed QRPA formalisms [21–25]. This is particularly the case of ^{150}Nd (^{150}Sm) that has received increasing attention in the last years because of the large phasespace factor and relatively short halflife, as well as for the large energy that will reduce the background contamination. ^{150}Nd is currently considered as one of the best candidates to search for the decay in the planned experiments SNO+, SuperNEMO, and DCBA.
The experimental information to constrain the calculations is not limited to the NMEs extracted from the measured halflives. We have also experimental information on the GamowTeller (GT) strength distributions of the single branches connecting the initial and final ground states with all the states in the intermediate nucleus. The GT strength distributions have been measured in both directions from () and () chargeexchange reactions (CER) and more recently from highresolution reactions, such as (, ^{2}He), (^{3}He, ), and (, ^{3}He) that allow us to explore in detail the lowenergy structure of the GT nuclear response in double decay partners [32–41]. In some instances there is also experimental information on the values of the decay of the intermediate nuclei.
Nuclear structure calculations are also constrained by the experimental occupation probabilities of neutrons and protons of the relevant singleparticle levels involved in the double decay process. In particular, the occupation probabilities of the valence shells , , , and for neutrons in ^{76}Ge and for protons in ^{76}Se have been measured in [42] and [43], respectively. The implications of these measurements on the double decay NMEs have been studied in [44–47].
In this paper we explore the possibility of describing all the experimental information available on the GT nuclear response within a formalism based on a deformed QRPA approach built on top of a deformed selfconsistent Skyrme HartreeFock calculation [48–51]. This information includes global properties about the GT resonance, such as its location and total strength, a more detailed description of the lowlying excitations, and decay NMEs. The study includes the decays , , , , and . This selection is motivated by recent highresolution CER experiments performed for ^{76}Ge(^{3}He, t) [39], ^{76}Se(d, ^{2}He)^{76}As [37], ^{128,130}Te(^{3}He, t)^{128,130}I [41], ^{116}Cd(p,n)^{116}In, and ^{116}Sn(n,p)^{116}In [40], as well as for ^{150}Nd(^{3}He, t)^{150}Pm, and ^{150}Sm(t, ^{3}He)^{150}Pm [38]. We also discuss on these examples the validity of the singlestate dominance (SSD) hypothesis [52] and the extended lowlyingstate dominance (LLSD) that includes the contribution of the lowlying excited states in the intermediate nuclei to account for the double decay rates.
The paper is organized as follows: In Section 2, we present a short introduction to the theoretical approach used in this work to describe the energy distribution of the GT strength. We also present the basic expressions of the decay. In Section 3 we present the results obtained from our approach, which are compared with the experimental data available. Section 4 contains a summary and the main conclusions.
2. Theoretical Approach
The description of the deformed QRPA approach used in this work is given elsewhere [22, 53–55]. Here we give only a summary of the method. We start from a selfconsistent deformed HartreeFock (HF) calculation with densitydependent twobody Skyrme interactions. Time reversal symmetry and axial deformation are assumed in the calculations [56]. Most of the results in this work are performed with the Skyrme force SLy4 [57], which is one of the most widely used and successful interactions. Results from other Skyrme interactions have been studied elsewhere [48–51, 58] to check the sensitivity of the GT nuclear response to the twobody effective interaction.
In our approach, we expand the singleparticle wave functions in terms of an axially symmetric harmonic oscillator basis in cylindrical coordinates, using twelve major shells. This amounts to a basis size of 364, the total number of independent deformed HO states. Pairing is included in BCS approximation by solving the corresponding BCS equations for protons and neutrons after each HF iteration. Fixed pairing gap parameters are determined from the experimental mass differences between even and odd nuclei. Besides the selfconsistent HF+BCS solution, we also explore the energy curves, that is, the energy as a function of the quadrupole deformation , which are obtained from constrained HF+BCS calculations.
The energy curves corresponding to the nuclei studied can be found in [50, 51, 58]. The profiles of the energy curves for ^{76}Ge and ^{76}Se exhibit two shallow local minima in the prolate and oblate sectors. These minima are separated by relatively lowenergy barriers of about 1 MeV. The equilibrium deformation corresponds to in ^{76}Ge and in ^{76}Se. We get soft profiles for ^{116}Cd with a minimum at and an almost flat curve in ^{116}Sn between and . We obtain almost spherical configurations in the ground states of ^{128}Te and ^{130}Te. The energies differ less than 300 keV between quadrupole deformations and . On the other hand, for ^{128}Xe and ^{130}Xe we get in both cases two energy minima corresponding to prolate and oblate shapes, differing by less than 1 MeV, with an energy barrier of about 2 MeV. The ground states correspond in both cases to the prolate shapes with deformations around . For ^{150}Nd and ^{150}Sm we obtain two energy minima, oblate and prolate, but with clear prolate ground states in both cases at and , respectively. We obtain comparable results with other Skyrme forces. The relative energies between the various minima can change somewhat for different Skyrme forces [50, 51, 58], but the equilibrium deformations are very close to each other changing at most by a few percent.
After the HF+BCS calculation is performed, we introduce separable spinisospin residual interactions and solve the QRPA equations in the deformed ground states to get GT strength distributions and decay NMEs. The residual force has both particlehole (ph) and particleparticle (pp) components. The repulsive ph force determines to a large extent the structure of the GT resonance and its location. Its coupling constant is usually taken to reproduce them [53–55, 59–62]. We use MeV. The attractive part is basically a protonneutron pairing interaction. We also use a separable form [55, 60, 61] with a coupling constant usually fitted to reproduce the experimental halflives [62]. We use in most of this work a fixed value MeV, although we will explore the dependence of the NMEs on in the next section. Earlier studies on ^{150}Nd and ^{150}Sm carried out in [24, 63] using a deformed QRPA formalism showed that the results obtained from realistic nucleonnucleon residual interactions based on the Brueckner matrix for the CDBonn force produce results in agreement with those obtained from schematic separable forces similar to those used here.
The QRPA equations are solved following the lines described in [53–55, 60, 61]. The method we use is as follows. We first introduce the protonneutron QRPA phonon operatorwhere and are quasiparticle creation and annihilation operators, respectively. labels the RPA excited state and its corresponding excitation energy, and and are the forward and backward phonon amplitudes, respectively. The solution of the QRPA equations is obtained by solving first a dispersion relation [55, 60, 61], which is of fourth order in the excitation energies . The GT transition amplitudes connecting the QRPA ground state () to one phonon states () are given in the intrinsic frame by where () are the BCS occupation amplitudes for neutrons and protons. Once the intrinsic amplitudes are calculated, the GT strength (GT) in the laboratory frame for a transition can be obtained asTo obtain this expression we have used the Bohr and Mottelson factorization [64, 65] to express the initial and final nuclear states in the laboratory system in terms of the intrinsic states. A quenching factor, , is applied to the weak axialvector coupling constant and included in the calculations. The physical reasons for this quenching have been studied elsewhere [10, 66, 67] and are related to the role of nonnucleonic degrees of freedom, absent in the usual theoretical models, and to the limitations of model space, manynucleon configurations, and deep correlations missing in these calculations. The implications of this quenching on the description of single and double decay observables have been considered in several works [12, 30, 68–71], where both the effective value of and the coupling strength of the residual interaction in the channel are considered free parameters of the calculation. It is found that very strong quenching values are needed to reproduce simultaneously the observations corresponding to the halflives and to the single decay branches. One should note however that the QRPA calculations that require a strong quenching to fit the NMEs were performed within a spherical formalism neglecting possible effects from deformation degrees of freedom. Because the main effect of deformation is a reduction of the NMEs, deformed QRPA calculations shall demand less quenching to fit the experiment.
Concerning the decay NMEs, the basic expressions for this process, within the deformed QRPA formalism used in this work, can be found in [21, 22, 72]. Deformation effects on the NMEs have also been studied within the projected HartreeFockBogoliubov model [27]. Attempts to describe deformation effects on the decay within QRPA models can also be found in [25, 73].
The halflife of the decay can be written aswhere are the phasespace integrals [74, 75] and the nuclear matrix elements containing the nuclear structure part involved in the process:In this equation are the QRPA intermediate states reached from the initial (final) nucleus. and are labels that classify the intermediate states that are reached from different initial and final ground states. The overlaps take into account the nonorthogonality of the intermediate states. Their expressions can be found in [21]. The energy denominator involves the energy of the emitted leptons, which is given on average by , as well as the excitation energies of the intermediate nucleus. In terms of the QRPA excitation energies the denominator can be written as where is the QRPA excitation energy relative to the initial (final) nucleus. It turns out that the NMEs are quite sensitive to the values of the denominator, especially for lowlying states, where the denominator takes smaller values. Thus, it is a common practice to use some experimental normalization of this denominator to improve the accuracy of the NMEs. In this work we also consider the denominator , which is corrected with the experimental energy of the first state in the intermediate nucleus relative to the mean groundstate energy of the initial and final nuclei, in such a way that the experimental energy of the first state is reproduced by the calculations:Running sums will be shown later for the two choices of the denominator, and . When the ground state in the intermediate nucleus of the double decay partners is a state, the energy is given bywhere and are the experimental energies of the decays of the intermediate nucleus into the parent and daughter partners, respectively. This is the case of ^{116}In and ^{128}I, which are both ground states. In the other cases, although the ground states in the intermediate nuclei are not states, the first excited states appear at a very low excitation energy; MeV in ^{76}As [39], MeV in ^{130}I [41], and MeV in ^{150}Pm [38]. Therefore, to a good approximation we also determine using (9).
The existing measurements for the decay halflives () have been recently analyzed in [9]. Adopted values for such halflives can be seen in Table 1. Using the phasespace factors from the evaluation [74] that involves exact Dirac wave functions including electron screening and finite nuclear size effects, we obtain the experimental NMEs shown in Table 1, for bare and quenched factors. It should be clear that the theoretical NMEs defined in (6) do not depend on the factors. Hence, the values obtained for the experimental NMEs extracted from the experimental halflives through (5) depend on the value used in this equation.

3. Results
3.1. GamowTeller Strength Distributions
The energy distributions of the GT strength obtained from our formalism are displayed in Figures 1 and 2. Figure 1 contains the strength distributions for ^{76}Ge, ^{116}Cd, ^{128}Te, ^{130}Te, and ^{150}Nd. The theoretical curves correspond to the calculated distributions folded with 1 MeV width BreitWigner functions, in such a way that the discrete spectra obtained in the calculations appear now as continuous curves. They give the GT strength per MeV and the area below the curves in a given energy interval gives us directly the GT strength contained in that energy interval. We compare our QRPA results from SLy4 obtained with the selfconsistent deformations with the experimental strengths extracted from CERs [34, 38, 40]. In the cases of ^{76}Ge, ^{128}Te, and ^{130}Te, the data from [34] includes the total GT measured strength of the resonances and their energy location. Namely, (GT) = 12.43 at MeV in ^{76}Ge, (GT) = 34.24 at MeV in ^{128}Te, and (GT) = 38.46 at MeV in ^{130}Te. We have folded these strengths with the same functions used for the calculations to facilitate the comparison. They can be seen with dashed lines in Figure 1.
Figure 2 contains the strength distributions corresponding to ^{76}Se, ^{116}Sn, ^{128}Xe, ^{130}Xe, and ^{150}Sm. The QRPA results folded with the same 1 MeV width BreitWigner functions are compared with the experimental strengths extracted from CERs [35–38, 40]. On the other hand, Figures 3 and 4 contain the accumulated GT strength in the low excitation energy. Figure 3 contains the same cases as in Figure 1 with additional highresolution data from [39] for ^{76}Ge and from [41] for ^{128,130}Te. Figure 4 contains the same cases as in Figure 2, but as accumulated strengths in the lowenergy range.
One should notice that the measured strength extracted from the cross sections contains two types of contributions that cannot be disentangled, namely, GT ( operator) and isovector spin monopole (IVSM) ( operator). Thus, the measured strength corresponds actually to (GT+IVSM). Different theoretical calculations evaluating the contributions from both GT and IVSM modes are available in the literature [38, 40, 76–78]. The general conclusion tells us that in the () direction the strength distribution below 20 MeV is mostly caused by the GT component, although nonnegligible contributions from IVSM components are found between 10 and 20 MeV. Above 20 MeV, there is no significant GT strength in the calculations. In the () direction the GT strength is expected to be strongly Pauli blocked in nuclei with more neutrons than protons and therefore the measured strength is mostly due to the IVSM resonance. Nevertheless, the strength found in lowlying isolated peaks is associated with GT transitions because the continuous tail of the IVSM resonance is very small at these energies and is not expected to exhibit any peak. In summary, the measured strength in the () direction can be safely assigned to be GT in the lowenergy range below 10 MeV and with some reservations between 10 and 20 MeV. Beyond 20 MeV the strength would be practically due to IVSM. On the other hand, the measured strength in the () direction would be due to IVSM transitions, except in the lowlying excitation energy below 23 MeV, where the isolated peaks observed can be attributed to GT strength. This is the reason why we plot experimental data in Figure 4 only up to 3 MeV.
In general terms, we reproduce fairly well the global properties of the GT strength distributions, including the location of the resonance and the total strength measured (see Figure 1). In the () direction, the strength is strongly suppressed (compare the vertical scales in Figures 1 and 2). As expected, a strong suppression of takes place in nuclei with a large neutron excess. The experimental information on strengths is mainly limited to the lowenergy region and it is fairly well reproduced by the calculations. The accumulated strengths in the lowenergy range shown in Figures 3 and 4 show more clearly the degree of accuracy achieved by the calculations. Although a detailed spectroscopy is beyond the capabilities of our model and the isolated transitions are not well reproduced by our calculations, the overall agreement with the total strength contained in this reduced energy interval, as well as with the profiles of the accumulated strength distributions, is satisfactory. In general, the experimental () shows spectra more fragmented than the calculated ones, but the total strength up to 3 MeV is well reproduced with the only exception of ^{116}Cd, where we obtain less strength than observed. The total measured () strength up to 3 MeV is especially well reproduced in the case of ^{150}Sm, whereas it is somewhat underestimated in ^{76}Se and overestimated in ^{116}Sn.
We can see in Figures 3 and 4 with blue dots the (GT) values extracted from the decays of the intermediate nuclei ^{116}In and ^{128}I. They can be compared with experimental results extracted from CERs, as well as with the theoretical calculations. The electron capture experiment on ^{116}In [79] gives s with a corresponding strength () = 0.402. The decay yields () = 0.256 [36]. The decay of ^{128}I yields () = 0.087 and () = 0.079 [41]. The sensitivity of these distributions to the effective interactions and to nuclear deformation was discussed in previous works [22, 48, 49, 51, 58, 72]. Different calculations [21, 24, 68, 78, 80] based also on QRPA formalisms with different degrees of sophistication agree qualitatively in the description of the single branches of double decay partners.
3.2. Double Decay
It is well known that the NMEs are very sensitive to the residual interactions, as well as to differences in deformation between initial and final nuclei [21, 22]. We show in Figure 5 the NMEs calculated with the selfconsistent deformations as a function of the coupling constant of the residual force for the decays of ^{76}Ge, ^{116}Cd, ^{128}Te, ^{130}Te, and ^{150}Nd. The shaded bands correspond to the experimental NMEs extracted from the measured halflives. For each nucleus the band is delimited by the lower and upper values obtained using bare () and quenched values, respectively (see Table 1). Results obtained with the energy denominator are displayed with solid lines, whereas results obtained with are shown with dashed lines. denominators produce in all cases larger NMEs than . We can see that the experimental NMEs contained in the shaded region are reproduced within some windows of the parameter . It is not our purpose here to get the best fit or the optimum value of that reproduces the experimental NMEs because this value will change by changing or the underlying mean field structure. In this work we take MeV as an approximate value that reproduces reasonably well the experimental information on both single branches and NMEs.
Figure 6 shows the running sums for the NMEs calculated with MeV. These are the partial contributions to the NMEs of all the states in the intermediate nucleus up to a given energy. Obviously, the final values reached by the calculations at 20 MeV in Figure 6 correspond to the values in Figure 5 at MeV. The final values of the running sums for other can be estimated by looking at the corresponding values in Figure 5. As in the previous figure, we also show the results obtained with denominators (solid) and (dashed). The main difference between them is originated at low excitation energies, where the relative effect of using shifted energies is enhanced. The effect at larger energies is negligible and we get a constant difference between and , which is the difference accumulated in the first few MeV. The contribution to the NMEs in the region between 10 and 15 MeV that can be seen in most cases is due to the GT resonances observed in Figure 1. This contribution is small because of the joint effects of large energy denominators in (6) and the mismatch between the excitation energies of the and resonances.
The running sums are very useful to discuss the extent to which the singlestate dominance hypothesis applies. This hypothesis tells us that, to a large extent, the NMEs will be given by the transition through the ground state of the intermediate oddodd nucleus in those cases where this ground state is a state reachable by allowed GT transitions. One important consequence of the SSD hypothesis would be that the halflives for decay could be extracted accurately from simple experiments, such as single and electron capture measurements of the intermediate nuclei to the ground states of the neighbor eveneven nuclei. Theoretically, the SSD hypothesis would also imply an important simplification of the calculations because, to describe the decay from ground state to ground state, only the wave function of the ground state of the intermediate nucleus would be needed. Because not all of the double decaying nuclei have ground states in the intermediate nuclei (only ^{116}In and ^{128}I in the nuclei considered here), the SSD condition is extended by considering the relative contributions of the lowlying excited states in the intermediate nuclei to the total NMEs. This is called lowlyingsinglestate dominance [72] and can be studied in all nuclei. From the results displayed in Figure 6 we cannot establish clear evidences for SSD hypothesis from our calculations. Nevertheless, it is also worth mentioning that our NMEs calculated up to 5 MeV already account for most of the total NME calculated up to 20 MeV. This result agrees qualitatively with other results obtained in different QRPA calculations [81–84].
The SSD hypothesis can be tested experimentally in the decays of ^{116}Cd and ^{128}Te where the intermediate nuclei have ground states. By measuring the two decay branches of ^{116}In and ^{128}I, the values of the ground state to ground state () can be extracted. From these values one can obtain the GT strength:with = 6289 s [85]. Finally the NME within SSD is evaluated as
One can also determine the NME running sums using the experimental (GT) extracted from CERs and using the same phases for the matrix elements if one can establish a onetoone correspondence between the intermediate states reached from parent and daughter. Then, one can construct the NMEs from the measured GT strengths and energies in the CERs in the parent and daughter partners:where is the excitation energy of the th state relative to the ground state of the intermediate nucleus. Experimental NMEs running sums have been determined along this line using experimental from CERs in [39] for ^{76}Ge, in [40] for ^{116}Cd, and in [38] for ^{150}Nd. In the case of ^{128,130}Te they have not been determined because of the lack of data in the () direction. They can be seen in Figure 6 under the label .
In the case of ^{76}Ge, the NMEs are constructed by combining the data from ^{76}Ge(^{3}He, t)^{76}As [39] with those for transitions from ^{76}Se(d, ^{2}He)^{76}As [37]. A large fragmentation of the GT strength was found in the experiment, not only at high excitation energies, but also at low excitation energy, which is rather unusual. In addition, a lack of correlation between the GT excitation energies from the two different branches was also observed. Thus, for the evaluation of the NMEs a onetoone connection between the and transitions leading to the excited state in the intermediate nucleus needs to be established. In particular, since the spectra from the two CER experiments had rather different energy resolutions, the strength was accumulated in similar bins to evaluate the NMEs [39]. The summed matrix element amounted to 0.186 up to an excitation energy of 2.22 MeV.
In the case of ^{116}Cd, ^{116}Cd()^{116}In and ^{116}Sn()^{116}In [40] CERs were used to evaluate the LLSD NMEs. The running sum starts at 0.14 at zero excitation energy and reaches a value of 0.31 at 3 MeV excitation energy. The value at zero energy can be compared with the value obtained by using the values of the decay in ^{116}In mentioned above. The value constructed in this way amounts to NME(SSD) = 0.168 [79]. In the case of ^{128}Te and ^{130}Te the lack of experimental information in the direction prevents us from evaluating the experimental LLSD estimates. However, an estimate of (SSD) = 0.019 in ^{128}Te can be obtained from the values of the decay in ^{128}I. Finally, in the case of ^{150}Nd, although the intermediate nucleus ^{150}Pm is not a state, assuming that the excited state at 0.11 MeV excitation energy observed in ^{150}Nd(^{3}He, t)^{150}Pm corresponds to all the GT strength measured between 50 keV and 250 keV in the reaction ^{150}Sm(t, ^{3}He)^{150}Pm, one obtains an estimate for the SSD (SSD) = 0.028 [38]. Extending the running sum by associating the corresponding GT strengths bins from the reactions in both directions and assuming a coherent addition of all the bins, one gets (SSD) = 0.13 [38] up to an excitation energy in the intermediate nucleus of 3 MeV. This experimental running sum is included in Figure 6. In all the cases, the experimental running sum is larger than the calculations and tends to be larger than the experimental values extracted from the halflives. However, one should always keep in mind that the present experimental LLSD estimates are indeed upper limits because the phases of the NMEs are considered always positive. Although the present calculations favor coherent phases in the lowenergy region, the phases could change depending on the theoretical model. In particular the sensitivity of these phases to the residual interaction has been studied in [63].
4. Summary and Conclusions
In summary, using a theoretical approach based on a deformed HF+BCS+QRPA calculation with effective Skyrme interactions, pairing correlations, and spinisospin residual separable forces in the and channels, we have studied simultaneously the GT strength distributions of the double decay partners (^{76}Ge, ^{76}Se), (^{116}Cd, ^{116}Sn), (^{128}Te, ^{128}Xe), (^{130}Te, ^{130}Xe), and (^{150}Nd, ^{150}Sm) reaching the intermediate nuclei ^{76}As, ^{116}In, ^{128}I, ^{130}I, and ^{150}Pm, respectively, as well as their NMEs. In this work we use reasonable choices for the twobody effective interaction, residual interactions, deformations, and quenching factors. The sensitivity of the results to the various ingredients in the theoretical model was discussed elsewhere.
Our results for the energy distributions of the GT strength have been compared with recent data from CERs, whereas the calculated NMEs have been compared with the experimental values extracted from the measured halflives for these processes, as well as with the running sums extracted from CERs.
The theoretical approach used in this work has been demonstrated to be well suited to account for the rich variety of experimental information available on the nuclear GT response. The global properties of the energy distributions of the GT strength and the NMEs are well reproduced, with the exception of a detailed description of the lowlying GT strength distributions that could clearly be improved. The NMEs extracted from the experimental halflives are also reproduced by the calculations with some overestimation (underestimation) in the case of ^{116}Cd (^{128}Te).
We have also upgraded the theoretical analysis of SSD and LLSD hypotheses and we have compared our calculations with the experimental running sums obtained by considering recent measurements from CERs and decays of the intermediate nuclei.
It will be interesting in the future to extend these calculations by including all the double decay candidates and to explore systematically the potential of this method. It will be also interesting to explore the consequences of the isospin symmetry restoration, as it was investigated in [86]. In HF+BCS and QRPA neither the ground states nor the excited states are isospin eigenstates, but the expectation values of the operator are conserved. This implies that in the () the transition operator connects states with a given expectation value of to states with expectation value of .
Competing Interests
The authors declare that they have no competing interests.
Acknowledgments
This work was supported by MINECO (Spain) under Research Grant no. FIS201451971P. O. Moreno acknowledges support from a Marie Curie International Outgoing Fellowship within the European Union Seventh Framework Programme, under Grant Agreement PIOFGA2011298364 (ELECTROWEAK).
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Copyright © 2016 P. Sarriguren et al. 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 SCOAP^{3}.