Advances in High Energy Physics
Volume 2016 (2016), Article ID 8417598, 8 pages
http://dx.doi.org/10.1155/2016/8417598

Research Article

Magnetic Hexadecapole Transitions and Neutrino-Nuclear Responses in Medium-Heavy Nuclei

Lotta Jokiniemi,¹ Jouni Suhonen,¹ and Hiroyasu Ejiri²

¹Department of Physics, University of Jyvaskyla, P.O. Box 35, 40014 Jyvaskyla, Finland
²Research Center for Nuclear Physics, Osaka University, Osaka 567-0047, Japan

Received 17 March 2016; Accepted 14 April 2016

Academic Editor: Enrico Lunghi

Copyright © 2016 Lotta Jokiniemi 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 SCOAP³.

Abstract.

Neutrino-nuclear responses in the form of squares of nuclear matrix elements, NMEs, are crucial for studies of neutrino-induced processes in nuclei. In this work we investigate magnetic hexadecapole (M4) NMEs in medium-heavy nuclei. The experimentally derived NMEs, (M4), deduced from observed M4 transition half-lives are compared with the single-quasiparticle (QP) NMEs, (M4), and the microscopic quasiparticle-phonon model (MQPM) NMEs (M4). The experimentally derived M4 NMEs are found to be reduced by a coefficient with respect to (M4) and by with respect to (M4). The M4 NMEs are reduced a little by the quasiparticle-phonon correlations of the MQPM wave functions but mainly by other nucleonic and nonnucleonic correlations which are not explicitly included in the MQPM. The found reduction rates are of the same order of magnitude as those for magnetic quadrupole transitions and Gamow-Teller (GT) and spin-dipole (SD) transitions. The impacts of the found reduction coefficients on the magnitudes of the NMEs involved in astroneutrino interactions and neutrinoless double beta decays are discussed.

1. Introduction

Neutrino interactions in nuclei are studied, for example, by investigating scatterings of astroneutrinos on nuclei and by the attempts to record the neutrinoless double beta () decays. Here the neutrino-nuclear responses can be condensed in the squares of nuclear matrix elements (NMEs) and it is necessary to study through them the neutrino properties and astroneutrino reactions that are of interest to particle physics and astrophysics, as discussed in review articles [1–4] and references therein.

The present work aims at investigating the magnetic hexadecapole (M4) NMEs, (M4), in medium-heavy nuclei to study higher-multipole axial-vector NMEs associated with higher-energy components of astroneutrino reactions and decays. Such components are shown to be important for, for example, the decays [5].

Neutrino-nuclear responses associated with neutral-current (NC) and charged-current (CC) interactions are studied by investigating the relevant and decay transitions or NC and CC scatterings on nuclei. The momenta involved in astroneutrino scatterings and decays are of the order of 50–100 MeV/c. Accordingly, depending on the involved momentum exchanges, the multipoles with angular momenta up to around 4-5 are involved (e.g., decays mediated by light Majorana neutrinos; see [5]), or even higher multipoles can be engaged ( decays mediated by heavy Majorana neutrinos; see [5]).

In some previous works, axial-vector CC resonances of GT(1⁺) and SD(2⁻) NMEs for allowed and first-forbidden transitions are shown to be reduced much in comparison with the quasiparticle (QP) and pnQRPA (proton-neutron quasiparticle random-phase approximation) NMEs [6–10] due to spin-isospin () nucleonic and nonnucleonic correlations and nuclear-medium effects. These studies show that exact theoretical evaluations for the astroneutrino and NMEs, including possible renormalization of the axial-vector coupling constant , are hard. The corresponding NC nuclear responses of magnetic dipole (M1) and quadrupole (M2) transitions are also known to be much reduced with respect to the QP NMEs [11]. Similar studies have been conducted in the case of the two-neutrino double beta decays in [12, 13] in the framework of the IBA-2 model. Also the derivation of effective operators has been proposed [14]. All these studies bear relevance to the previously mentioned Majorana-neutrino mediated decays, to high-energy astroneutrino reactions, but also to the lower-energy (up to 30 MeV) supernova-neutrino scatterings off nuclei, as shown, for example, in [15–18].

In the light of the above discussions it is of great interest to investigate the spin-hexadecapole (4⁻) NMEs to see how the higher-multipole NMEs are reduced by the nucleonic and nonnucleonic spin-isospin correlations. Actually, there are almost no experimental CC hexadecapole NMEs in medium-heavy nuclei since the decays are very rare third-forbidden unique transitions. However, it turns out that there are few measurements of the half-lives and electron spectra of the more complex fourth-forbidden nonunique transitions and they can serve as potential testing grounds concerning the quenching effects of the weak vector () and axial-vector () coupling constants [19]. On the other hand, there are many experimental data on NC M4 NMEs, where the isovector component of the NME is related to the analogous NME on the basis of the isospin symmetry. Thus we discuss mainly the M4 transitions in the present report with the aim of helping evaluate/confirm, for example, the NMEs concerning their higher-multipole aspects.

2. Experimental M4 NMEs

Here we discuss stretched M4 transitions with , where and are the initial and final state spins and . The M4 transition rate (per sec) is given in terms of the reduced M4 strength (M4) as [20]

where is the ray energy in units of MeV and is the conversion-electron coefficient. The reduced strength is expressed in terms of the M4 NME in units of as

The M4 NME is expressed in terms of the M4 coupling constants (M4) and the M4 matrix element (M4) as

where the first and the second terms are for the odd-proton () and odd-neutron () transition NMEs with being the isospin component ( for neutron and for proton). The coupling constant is written as

where for proton and for neutron, and are the proton and neutron magnetic moments, and and are the proton and neutron orbital coefficients. The M4 matrix element is expressed as

where is the nuclear radius and is the spherical harmonic for multipole .

The isotopes used for ongoing and/or future experiments are , , , , , , and [2]. They are in the mass regions of = 70–120 and = 130–150. The single-quasiparticle (single-QP) M4 transitions in these mass regions are uniquely tagged by the pairs and , respectively. Here the higher spin state is the intruder one from the higher major shell with opposite parity. The single-particle M4 NMEs corresponding to these tagging transitions are quite large because of the large radial and angular overlap integrals.

The single-quasiparticle M4 transitions in the mentioned two mass regions are analyzed in Tables 1 and 2. The M4 NMEs derived from the experimental half-lives are given in the third column of these tables.

Table 1: (M4) NMEs for M4 transitions in the mass region of = 70–, where the major single-QP transition is -. Here stands for the odd-proton/odd-neutron transition. , , and are the experimental, single-QP, and MQPM NMEs in units of 10³ fm³.

Nucleus
Transition

Kr

0.528
1.57
1.44

Y

0.739
2.12
2.02

Zr

0.559
1.60
1.47

Y

0.480
2.13
1.83

In

0.706
2.38
2.09

In

0.670
2.40
2.13

In

0.640
2.33
2.10

In

0.609
2.45
2.03

In

0.603
2.46
2.05

In

0.614
2.48
2.03

Table 2: The same as Table 1 for = 130–150, where the major single-quasiparticle transition is -.

Nucleus
Transition

Xe

1.11
3.12
2.87

Ba

1.03
3.13
2.77

Ba

0.968
3.12
2.82

Nd

0.893
3.17
2.79

Sm

0.878
3.19
2.81

The values of (M4) are plotted against the mass number in Figure 1. They are around and for the two mass regions, respectively. They are well expressed as

where the mass number reflects the dependence of the M4 NME.

(a)

(b)

Figure 1: (a) EXP: experimental NMEs (M4) for odd-neutron transitions (light-blue squares) and odd-proton transitions (dark-blue diamonds). QP: quasiparticle NMEs (M4) for odd-neutron transitions (light-blue tip-up triangles) and odd-proton transitions (dark-blue tip-down triangles). (b) EXP: experimental NMEs (M4) for odd-neutron transitions (light-blue squares) and odd-proton transitions (dark-blue diamonds). MQPM: NMEs (M4) for odd-neutron transitions (light-blue tip-up triangles) and odd-proton transitions (dark-blue tip-down triangles).

3. Quasiparticle M4 NMEs

The M4 transitions given in Tables 1 and 2 are all, in their simplest description, transitions between single-quasiparticle states. The NMEs for the single-quasiparticle transitions are written by using the single-particle matrix element (M4) and the pairing coefficient as

where the pairing coefficient is given by

and () and () are the vacancy and occupation amplitudes for the initial (final) state. The single-quasiparticle states discussed here are low-lying states located at the diffused Fermi surface, as shown in Figure 2. Thus the occupation and vacancy probabilities are in the region of , and the pairing coefficient is given roughly as . In this work the single-quasiparticle NMEs (M4) are calculated by using the BCS wave functions with HO single-particle states. They are given in the fifth column of Tables 1 and 2 and are plotted in Figure 1(a).

Figure 2: Schematic diagram of the energy () and the occupation probabilities, and , for the initial and final states (see body of text). The energy levels are shown by the horizontal lines. Vacancy probabilities are given as and . The paring coefficient for the transition is given by .

The experimental M4 matrix elements (M4) are uniformly smaller by a coefficient of around 0.29 ± 0.05 than the single-quasiparticle ones, (M4). We introduce a reduction coefficient as in the case of GT(1⁺) and SD(2⁻) [8, 10] transitions. It is defined as

where , with , are the reduction coefficients for single quasi-proton and quasi-neutron M4 transitions, respectively. The ratios are and , as shown in Figure 3(a). The found reductions are consistent with the reductions discussed in [11].

(a)

(b)

Figure 3: Reduction coefficients for the M4 NMEs. (a) : ratios of experimental NMEs (M4) to the quasiparticle NMEs (M4) for odd-neutron transitions (light-blue squares) and odd-proton transitions (dark-blue diamonds). (b) : ratios of experimental NMEs (M4) to the MQPM NMEs (M4) for odd-neutron transitions (light-blue squares) and for odd-proton transitions (dark-blue diamonds).

The quasiparticle NMEs (M4) are calculated by assuming a stretched M4 transition between the initial and final nuclear states (see column 2 of Tables 1 and 2) that are assumed to have a one-quasiparticle structure. These states are thus described as

where creates a quasiparticle on a nuclear mean-field orbital with quantum numbers , where contains the principal quantum number , the orbital angular momentum (), and total angular momentum () quantum numbers in the form as displayed in column 2 of Tables 1 and 2. Here is the projection of the total angular momentum and is the BCS vacuum. The quasiparticles are defined by the Bogoliubov-Valatin transformation as

where is the particle creation operator and the time-reversed particle annihilation operator is defined by with . The and coefficients are the vacancy and occupation amplitudes present also in the quasiparticle matrix elements of (7) and (8). The values of these amplitudes are obtained in BCS calculations (for details see, e.g., [21]) and they are used also in the subsequent nuclear-structure calculations of the odd-mass nuclei and their neighboring even-even-mass reference nuclei.

4. Microscopic Quasiparticle-Phonon Model for M4 NMEs

The microscopic quasiparticle-phonon model (MQPM) takes the structure of the nuclear states beyond the approximation (10). In the MQPM this extension is done in the traditional way of starting from an even-even reference nucleus where the states are described as QRPA (quasiparticle random-phase approximation) states called here phonons since the lowest ones are usually collective vibrational states. These states can be formally written as

where the phonon operator creates a nuclear state with quantum numbers , containing the angular momentum , parity , and the quantum number which enumerates states with the same angular momentum and parity. The state (12) is a linear combination of two-quasiparticle states as explicitly written in [22] where the MQPM was first introduced. To arrive at a state in the neighboring odd-mass nucleus one has to couple a proton (proton-odd nucleus) or a neutron (neutron-odd nucleus) quasiparticle to the phonon operator which is a two-quasiparticle operator. In this way one creates three-quasiparticle states in the traditional quasiparticle-phonon coupling scheme and these states are then mixed with the one-quasiparticle states by the residual nuclear Hamiltonian (for details see [22]). Hence we obtain the MQPM states

where a th state of angular momentum and its projection is created in an odd-mass nucleus by a creation operator which mixes one-quasiparticle and three-quasiparticle components in the form

where the first term is the one-quasiparticle contribution and the second term is the quasiparticle-phonon contribution. The amplitudes and are computed from the MQPM equations of motion [22]. In solving these equations special care is to be taken to handle the overcompleteness and the nonorthogonality of the quasiparticle-phonon basis, as described in detail in [22].

In the actual calculations we used slightly modified Woods-Saxon single-particle energies to improve the quality of the computed energy spectra of the odd-mass nuclei involved in the present work. This resulted in a good correspondence between the computed and experimental low-energy spectra of these nuclei. We adopted a residual Hamiltonian with realistic effective two-nucleon interactions derived from the Bonn-A one-boson-exchange potential [23]. The free parameters of the interaction were fixed in the BCS and QRPA phases of the calculations as explained in [24, 25]. The two-body monopole matrix elements were multiplied by one parameter for protons and one for neutrons to scale phenomenologically the proton and neutron pairing strengths separately. This was done by fitting the computed pairing gaps to the phenomenological ones, derived from the measured proton and neutron separation energies [26]. The QRPA step contained two parameters for each multipole to control the energies of the even-even excited states. These were the strengths of the particle-hole and particle-particle parts of the two-nucleon interaction. The particle-hole interaction controls the energies of collective states and thus it was fitted to reproduce the experimental excitation energy of the lowest state of a given multipolarity , whenever data existed. When no data was available the bare -matrix was used in the calculations. Also the particle-particle part of the multipole interaction was kept as bare -matrix interaction.

After performing the BCS and QRPA calculations in the reference even-even nuclei, the initial and final nuclear states in the neighboring odd-mass nuclei, of interest in the present work, were formed by first creating the quasiparticle-phonon components of the operator (14). The convergence of the MQPM results for the energies of the involved states and the M4 transition amplitudes between them were monitored by adding more and more QRPA phonons of different multipolarities in the diagonalization of the residual Hamiltonian. In terms of the cut-off energy of the added phonons the convergence was achieved at around 14 MeV.

The converged M4 results are given in the sixth column of Tables 1 and 2 and are plotted in Figures 1(b) and 3(b). It is seen that the experimental M4 matrix elements, (M4), are uniformly smaller, by a coefficient around 0.33, than the MQPM NMEs (M4). Actually, the MQPM NMEs (M4) are 10–20% smaller than the QP NMEs (M4), as shown in Figure 4. The admixtures of the quasiparticle-phonon components in the wave functions (14) of the M4 initial and final states reduce the M4 NMEs a little, but not nearly enough to bring the MQPM NMEs close to the corresponding experimental ones, at least by using the bare coefficients (4) adopted in the present work. Hence, the major part of reduction from the MQPM NME to the experimental one (a reduction coefficient of 0.3) is considered to be due to such nucleonic and nonnucleonic correlations and nuclear-medium effects that are not explicitly included in the (traditional) quasiparticle-phonon coupling scheme that MQPM uses, that is, the even-even nucleus serving as a reference for the odd-mass one.

Figure 4: Ratios of the quasiparticle NMEs (M4) to the MQPM NMEs (M4) for odd-neutron transitions (light-blue squares) and odd-proton transitions (dark-blue diamonds).

5. Reduction of the Axial-Vector NMEs

The NME is decomposed into the isovector and isoscalar ones as [11]

where is and for an odd-proton and odd-neutron transition, respectively, and and are the isovector and isoscalar coupling constants. They are written as

with and .

The proton, neutron, isovector, and isoscalar M4 coupling constants are given as

where is the M4 coupling coefficient.

The M4 NMEs in (15) are rewritten as with , the symbols standing for the proton, neutron, isovector, and isoscalar components, respectively. Then the reduction coefficients and the weak couplings for proton and neutron transitions are expressed in terms of those for the isovector and isoscalar components as [11]

After this the isovector and isoscalar reduction coefficients can be derived as

Since the experimentally derived NMEs for the proton and neutron transitions are approximately the same, that is, , we get from (19) . The isovector M4 NMEs are reduced by the coefficient , in the same way as the M4 transition NMEs. It is notable that the amount of reduction for the isovector 4⁻   NMEs is the same as that found for the GT(1⁺) and SD(2⁻) decay NMEs [8, 10].

Axial-vector and NMEs for low-lying states are much reduced with respect to the QP NMEs due to the strong repulsive interactions since the axial-vector strengths are pushed up into the giant-resonance (GR) and the -isobar regions. The M4 reduction coefficient of is nearly the same as the coefficient for M2 transitions and and in the GT(1⁺) and SD(2⁻) decay NMEs, respectively [8, 10]. These reduction coefficients are plotted in Figure 5 with denoting the angular momentum content of the transition operator.

Figure 5: Reduction coefficients for the multipolarity () and () transitions (dark-blue diamonds) and those for () and () transitions (light-blue squares) in medium-heavy nuclei. Here denotes the transition angular momentum. The dotted line shows .

It seems that the reduction coefficients of the axial-vector NMEs are universal for NC and CC NMEs and for the angular momenta of = 1–4. The reduction is considered to be due to such polarization interactions and nuclear-medium effects that are not explicitly included in the models. Then the reduction rate ≈ 0.2–0.3, with respect to the QP NME, is expressed as [8, 10]

where and stand for the reductions due to the nucleonic polarization effects and nonnucleonic -isobar and nuclear-medium effects, respectively.

These universal effects may be represented by the effective weak coupling , depending on the model NME, to incorporate the effects that are not explicitly included in the nuclear-structure model. In case of the pnQRPA with explicit nucleonic correlations, one may use , while in the case of the QP model, without any correlations, , both in units of the bare value of .

Here we note that the repulsive interaction concentrates the strength to the highly excited GR, resulting in the reduction of the NMEs for low-lying states. Such reduction effect is incorporated in the pnQRPA with the strong interaction, so that the reduction factor is improved from to . On the other hand, such strong interaction to give rise to the possible M4 GR is not explicitly incorporated in the MQPM, and thus the reduction factor is only a little improved from to .

6. Discussion and Conclusions

Among other models, the QRPA-based models are used to compute the NMEs of double beta decays [4, 27]. In these calculations the importance of the quenching of magnifies since the NME includes the axial-vector NME proportional to the square of . The M4 NC results of the present investigation, together with the earlier M2 NC and GT and SD CC results, suggest that many of the leading multipoles in the decomposition of the neutrinoless NMEs are quenched roughly by the same amount by the correlations of the region as well as other nuclear-medium effects. Since the corresponding investigations have been done using data on low-lying nuclear states it is safe to say that the quenching applies at least to the low-lying states in nuclei. These observations are very relevant for the two-neutrino decays since they are low-energy phenomena and usually involve only one or few lowest states in the intermediate nucleus [1, 28, 29]. A consistent description of these decays can be achieved by using the quenched derived from the GT decays [30].

Actually, the observed single GT NMEs are reduced by the effective coupling constant with respect to the model NME, and thus the observed NMEs are well reproduced by using the experimental , that is, the experimental single NMEs for low-lying states [1, 2, 31]. However, it should be kept in mind that these results, important as such, cannot be directly applied to the processes since there large momentum exchanges are involved and also vector-type of NMEs and higher excited states contribute. In this case it is a big challenge to develop such nuclear models for the axial-vector weak processes that include explicitly appropriate nucleonic and nonnucleonic correlations. If successful, then in such models one could use the axial weak coupling of and be free from the uncertainties introduced by the effective (quenched) .

Neutrino-nucleus scatterings are important to probe many astrophysical phenomena, like the solar and supernova neutrinos [1, 32, 33]. The GT NMEs bring in most of the contributions for solar neutrinos and low-energy supernova neutrinos for neutrino energies below 15 MeV (see, e.g., [16, 17]). The SD NMEs play a role for medium-energy neutrinos above 15 MeV. For the low-energy solar neutrinos reliable calculations of the GT NMEs are needed to evaluate the SNU values for the pp, , CNO, and other neutrinos. Experimental GT strengths can also be used, if available [1]. The SD contributions can be important for the CC supernova antineutrino scatterings off nuclei even at low energies, as shown in [15–18].

The supernova-neutrino nucleosyntheses are sensitive to the neutrino CC and NC interactions, as discussed in a review article [33]. Here SD and higher-multipole NMEs are involved in the high-energy components of the supernova neutrinos. It is important for accurate evaluations of the isotope distributions to use appropriate NMEs and effective weak couplings of and . QRPA calculations were made for nuclei in [34].

The involved GT and SD NMEs can be studied via beta decays in nuclei where beta decay data is available. In some of these studies a strong quenching of both and has been conjectured [35–38]. Such quenching for the higher multipoles is extremely hard to study, the present study being a rather unique one in this respect. Quenching of the higher multipoles can also be studied via high-forbidden beta decays [19] but the available data is extremely scarce at the moment. Perspectives for the studies of the quenching of both and are given by the spectrum-shape method introduced in [19]. There the shape of the beta spectrum of the high-forbidden nonunique beta decays has been studied for the determination of the possible quenching of the weak constants. Use of this method can be boosted by future high-sensitive measurements of electron spectra in underground laboratories.

Finally, it is worth pointing out that the universal reduction/quenching of the NME, including , is related to the shift of the strength to the higher GR and isobar regions. Charge-exchange reactions report about a 50–60% of the GT sum rule (the Ikeda sum rule) up to GT GR, while the reactions claim that around 90% of the GT sum-rule strength is seen by including the strength beyond the GT GR up to 50 MeV [39]. Very careful investigations of the GT, SD, and higher-multipole strength distributions, by using charge-exchange reactions, are called for to see if the reduction/quenching of the strengths is partly due to the nonnucleonic () correlations [8, 20]. These investigations not only are interesting from the point of view of the double beta decay but also touch the projected double charge-exchange reactions [40] where the high-momentum response of nuclei is also probed.

Competing Interests

The authors declare that they have no competing interests.

Acknowledgments

This work was supported by the Academy of Finland under the Finnish Center of Excellence Program 2012–2017 (Nuclear and Accelerator Based Program at JYFL).

References

H. Ejiri, “Nuclear spin isospin responses for low-energy neutrinos,” Physics Reports, vol. 338, no. 3, pp. 265–351, 2000.

J. D. Vergados, H. Ejiri, and F. Šimkovic, “Theory of neutrinoless double-beta decay,” Reports on Progress in Physics, vol. 75, no. 10, Article ID 106301, 2012.

F. T. Avignone, S. R. Elliott, and J. Engel, “Double beta decay, Majorana neutrinos, and neutrino mass,” Reviews of Modern Physics, vol. 80, no. 2, pp. 481–516, 2008.

J. Suhonen and O. Civitarese, “Weak-interaction and nuclear-structure aspects of nuclear double beta decay,” Physics Report, vol. 300, no. 3-4, pp. 123–214, 1998.

J. Hyvärinen and J. Suhonen, “Nuclear matrix elements for 0ββ decays with light or heavy Majorana-neutrino exchange,” Physical Review C, vol. 91, no. 2, Article ID 024613, 2015.

A. Faessler, G. L. Fogli, E. Lisi, V. Rodin, A. M. Rotunno, and F. Šimkovic, “Overconstrained estimates of neutrinoless double beta decay within the QRPA,” Journal of Physics G: Nuclear and Particle Physics, vol. 35, no. 7, Article ID 075104, 2008.

J. Suhonen and O. Civitarese, “Probing the quenching of gA by single and double beta decays,” Physics Letters B, vol. 725, no. 1–3, pp. 153–157, 2013.

H. Ejiri, N. Soukouti, and J. Suhonen, “Spin-dipole nuclear matrix elements for double beta decays and astro-neutrinos,” Physics Letters B, vol. 729, pp. 27–32, 2014.

J. Suhonen and O. Civitarese, “Single and double beta decays in the A = 100, A = 116 and A = 128 triplets of isobars,” Nuclear Physics A, vol. 924, pp. 1–23, 2014.

H. Ejiri and J. Suhonen, “GT neutrino-nuclear responses for double beta decays and astro neutrinos,” Journal of Physics G: Nuclear and Particle Physics, vol. 42, no. 5, Article ID 055201, 2015.

H. Ejiri and J. I. Fujita, “Effective coupling constants for beta and gamma transitions in medium and heavy nuclei,” Physics Reports, vol. 38, no. 2, pp. 85–131, 1978.

J. Barea, J. Kotila, and F. Iachello, “Nuclear matrix elements for double-β decay,” Physical Review C, vol. 87, no. 1, Article ID 014315, 2013.

J. Barea, J. Kotila, and F. Iachello, “0ββ and 2ββ nuclear matrix elements in the interacting boson model with isospin restoration,” Physical Review C, vol. 91, no. 3, Article ID 034304, 2015.

J. D. Holt and J. Engel, “Effective double-β-decay operator for ⁷⁶Ge and ⁸²Se,” Physical Review C, vol. 87, no. 6, Article ID 064315, 7 pages, 2013.

C. Volpe, N. Auerbach, G. Colò, and N. Van Giai, “Charged-current neutrino-²⁰⁸Pb reactions,” Physical Review C, vol. 65, no. 4, Article ID 044603, 2002.

W. Almosly, E. Ydrefors, and J. Suhonen, “Neutral- and charged-current supernova-neutrino scattering off ¹¹⁶Cd,” Journal of Physics G: Nuclear and Particle Physics, vol. 40, no. 9, Article ID 095201, 2013.

W. Almosly, E. Ydrefors, and J. Suhonen, “Neutrino scattering off the stable cadmium isotopes: II. Charged-current processes,” Journal of Physics G: Nuclear and Particle Physics, vol. 42, no. 9, Article ID 095106, 2015.

R. Lazauskas and C. Volpe, “Neutrino beams as a probe of the nuclear isospin and spin-isospin excitations,” Nuclear Physics A, vol. 792, no. 3-4, pp. 219–228, 2007.

M. Haaranen, P. C. Srivastava, and J. Suhonen, “Forbidden nonunique β decays and effective values of weak coupling constants,” Physical Review C, vol. 93, no. 3, Article ID 034308, 2016.

A. Bohr and B. R. Mottelson, Nuclear Structure Volume I, II, Benjamin, New York, NY, USA, 1969, 1975.

J. Suhonen, From Nucleons to Nucleus: Concepts of Microscopic Nuclear Theory, Theoretical and Mathematical Physics, Springer, Berlin, Germany, 2007.

J. Toivanen and J. Suhonen, “Microscopic quasiparticle-phonon description of odd-mass isotopes and their β decay,” Physical Review C, vol. 57, no. 3, pp. 1237–1245, 1998.

K. Holinde, “Two-nucleon forces and nuclear matter,” Physics Reports, vol. 68, no. 3, pp. 121–188, 1981.

J. Suhonen, A. Faessler, T. Taigel, and T. Tomoda, “Suppression of the β ⁺-decays of ¹⁴⁸Dy, ¹⁵⁰Er and ¹⁵²Yb,” Physics Letters B, vol. 202, no. 2, pp. 174–178, 1988.

J. Suhonen, T. Taigel, and A. Faessler, “pnQRPA calculation of the β ⁺/EC quenching for several neutron-deficient nuclei in mass regions –110 and –156,” Nuclear Physics A, vol. 486, no. 1, pp. 91–117, 1988.

G. Audi, F. G. Kondev, M. Wang et al., “The Nubase2012 evaluation of nuclear properties,” Chinese Physics C, vol. 36, no. 12, p. 1157, 2012.

J. Suhonen and O. Civitarese, “Double-beta-decay nuclear matrix elements in the QRPA framework,” Journal of Physics G: Nuclear and Particle Physics, vol. 39, no. 8, Article ID 085105, 2012.

M. Bhattacharya, A. García, M. M. Hindi et al., “Electron capture decay of ¹¹⁶In and nuclear structure of double β decays,” Physical Review C, vol. 58, no. 2, p. 1247, 1998.

O. Civitarese and J. Suhonen, “Systematic study of the single-state dominance in 2νββ decay transitions,” Nuclear Physics A, vol. 653, no. 3, pp. 321–337, 1999.

P. Pirinen and J. Suhonen, “Systematic approach to β and 2νββ decays of mass nuclei,” Physical Review C, vol. 91, no. 5, Article ID 054309, 2015.

H. Ejiri, “Experimental nuclear matrix elements for two neutrino double beta decays and single beta decays,” Journal of the Physical Society of Japan, vol. 78, no. 7, Article ID 074201, 2009.

S. E. Woosley, D. H. Hartman, R. D. Hoffman, and W. C. Haxton, “The neutrino-process,” The Astrophysical Journal, vol. 356, pp. 272–301, 1990.

K. Langanke and G. Martínez-Pinedo, “Nuclear weak-interaction processes in stars,” Reviews of Modern Physics, vol. 75, no. 3, pp. 819–862, 2003.

M.-K. Cheoun, E. Ha, T. Hayakawa et al., “Neutrino induced reactions for -process nucleosynthesis of ⁹²Nb and ⁹⁸Tc,” Physical Review C, vol. 85, no. 6, Article ID 065807, 12 pages, 2012.

E. K. Warburton, “Core polarization effects on spin-dipole and first-forbidden β-decay operators in the lead region,” Physical Review C, vol. 42, no. 6, pp. 2479–2486, 1990.

E. K. Warburton, “First-forbidden β decay in the lead region and mesonic enhancement of the weak axial current,” Physical Review C, vol. 44, no. 1, pp. 233–260, 1991.

T. Suzuki, T. Yoshida, T. Kajino, and T. Otsuka, “β decays of isotones with neutron magic number of and r-process nucleosynthesis,” Physical Review C, vol. 85, no. 1, Article ID 015802, 2012.

Q. Zhi, E. Caurier, J. J. Cuenca-García, K. Langanke, G. Martínez-Pinedo, and K. Sieja, “Shell-model half-lives including first-forbidden contributions for r-process waiting-point nuclei,” Physical Review C, vol. 87, no. 2, Article ID 025803, 2013.

T. Wakasa, H. Sakai, H. Okamura et al., “Gamow-Teller strength of ⁹⁰Nb in the continuum studied via multipole decomposition analysis of the ⁹⁰Zr(p,n) reaction at 295 MeV,” Physical Review C, vol. 55, no. 6, p. 2909, 1997.

F. Cappuzzello, M. Cavallaro, C. Agodi et al., “Heavy-ion double charge exchange reactions: a tool toward nuclear matrix elements,” The European Physical Journal A, vol. 51, article 145, 2015.