# Competition of different coupling schemes in atomic nuclei

###### Abstract

Shell model calculations reveal that the ground and low-lying yrast states of the nuclei Pd and Cd are mainly built upon isoscalar spin-aligned neutron-proton pairs each carrying the maximum angular momentum allowed by the shell which is dominant in this nuclear region. This mode of excitation is unique in nuclei and indicates that the spin-aligned pair has to be considered as an essential building block in nuclear structure calculations. In this contribution we will discuss this neutron-proton pair coupling scheme in detail. In particular, we will explore the competition between the normal monopole pair coupling and the spin-aligned coupling schemes. Such a coupling may be useful in elucidating the structure properties of and neighboring nuclei.

The low-lying structures of many nuclei can be understood as the outcome of the competition between the pairing (or seniority) coupling scheme and the aligned coupling of individual particles in a non-spherical average potential. The seniority coupling dominates the low-lying states of semi-magic nuclei, where the driving force behind is the strong pairing interaction between like particles. Meanwhile, many open-shell nuclei have quadrupole moments that are much larger than could be attributed to a single particle, which implies the sharing of angular momentum between many particles. A remarkable feature of nuclear structure physics is that essential ingredients of the single-particle model could be retained by assuming that the nucleons move in an average nuclear field deviates from spherical symmetry, which removes the spurious degrees of freedom corresponding to the collective spectrum [1]. The transition between there two couplings in open-shell nuclei is expected to be rather fast [2, 3, 4].

Near the line, nuclear collectivity may be further enhanced by the interactions arising between neutrons and protons occupying orbitals with the same quantum numbers, which can form pairs with angular momenta to and isospin quantum numbers (isoscalar) and (isovector). The isovector channel manifests itself in a fashion similar to like-nucleon correlations. There has been longstanding and intensive interest in exploring the signature of isoscalar pairing (in particular pairs with and ) in the structure of self-conjugate nuclei [5, 6, 7, 8, 9, 10]. Possible fingerprints may be inferred from the delayed alignments in the ground-state rotational bands of deformed nuclei, but it is still controversial. In this contribution we would like to discuss the so-called spin-aligned neutron-proton pair coupling from a nuclear shell-model perspective. In some spherical nuclei it may overcome the normal pairing as the dominant coupling scheme of the ground state structure. We will show that the aligned pairs can generate striking regular evolution patterns in the energy spectra and transition probabilities along the yrast states of nuclei. These may be deemed as a new kind of collective mode with isoscalar character that is unique in the atomic nucleus. In a recent work the low-lying yrast states in Pd were observed and it was inferred that for the first time a transition from the isovector pair coupling mode to such spin-aligned coupling scheme may have occurred [11, 12]. For related earlier works, see Refs. [13, 14, 15, 16, 17].

I would like to remind you that, as one would expect, near the closed shell nucleus Sn, i.e., in Pd (Cd) with four (two) proton holes outside of Sn, the positions of the energy levels correspond to a pairing spectrum, as can be seen from Fig. 1 of Ref. [12] and Fig. 1. When the number of neutron holes increases, the levels tend to be equally separated, which is a characteristic of vibrational spectra. This are specially the cases for Pd and Cd which show equally-spaced level schemes up to and , respectively. Already the systematics of experimental data suggests gradual decrements in both the quadrupole deformation and ratio in nuclei when approaching the Sn shell closure [18, 19]. Many open shell nuclei, like Ru shown in Fig. 1, exhibit rotational-like ground state bands. The nuclei Sr and Zr are the most deformed ones in this region.

\brSpace | ||||||||||
---|---|---|---|---|---|---|---|---|---|---|

\mr | 0 | 1.458 | 2.283 | 2.549 | 2.688 | 1.220 | 1.592 | 1.882 | 1.930 | 0.626 |

-2.089 | -0.919 | -0.094 | 0.172 | 0.311 | -1.038 | -0.785 | -0.495 | -0.447 | -1.751 | |

-1.691 | -0.959 | -0.087 | 0.152 | 0.269 | -1.138 | -0.599 | -0.383 | -0.561 | -2.207 | |

\br |

To understand the yrast structures of Pd, Cd and neighboring nuclei, we perform nuclear shell model calculations within the (), () and model spaces using the Hamiltonian given in Ref. [21] and a variety of other interactions which are quoted therein. In particular, we perform calculations using as single-particle states the orbits and , with the interactions of Refs. [22, 23, 24], in order to explore the importance of configuration mixing in determining the structure of the spectrum.

In Table 1 we compare the strengths of the interaction matrix elements corresponding to different shell model spaces [21, 22, 24]. In the case of space, only the relative strengths are given for simplicity. The absolute strength of the monopole centroid has no influence on the coupling of the wave functions and excitation energies. Also it should be mentioned that the relative strength of the and monopole interactions does not play any role on the structure of nuclear states. That is, the wave functions remain unchanged by adding a constant to the or 1 part of the interaction. This modification only affects the relative energies of the states with different isospin quantum numbers.

The matrix element for the model space, for which we took from Ref. [21], are defined in the particle-particle channel by assuming Ni as the core. The mass dependence of the interaction is assumed to be for where is the mass number of the nucleus to be calculated. For we take the single-hole energies (relative to that of ) of MeV, MeV, MeV and MeV.

The calculated results for Ru and Cd isotopes are plotted in Fig. 1. Calculations are done with the shell-model code described in Ref. [25]. Calculations for the spectra of Pd isotopes could be found in Refs. [11, 12]. Present shell model calculations are able to include a large number of shells with the help of modern computers. In Fig. 2 we calculated the average number of holes in each orbitals of the model space in which four orbitals are involved. It is thus seen that it is the shell that dominates the occupancy. Also comparison with and calculations tend to suggest that many properties of nuclei in this region can be explained by calculations restricted the the single shell only. This does not mean that the other shells (the orbitals and even other higher lying shells) has no contribution to the wave function. But normally one may safely expect the effect from these shells can be taken into account through the renormalization of the effective interaction and effective operators (c.f., Table 1). The contributions from other shells may be deemed as the background whose effect on the nuclear structure is hard to identify. This is because our knowledge of complex objects like atomic nuclei are obtained through systematic studies of neighboring states. As a result, only relevant degrees of freedom that distinguish one state from the others can be identified. Simple models are only for us to understand the physics and the residual degrees of freedom. The real situation can be much more complex. Even the shell-model single-particle orbitals are very complicated from a microscopic point of view and can be very different from the real single-particle wave functions of the nucleus [26, 27]. Thus the shell occupancy plotted in Fig. 2 is a model dependent quantity. Also full shell model calculation has been feasible for the nucleus Cr since almost 20 years ago. But it is realized that the and shells would be enough to explain the bulk properties of this deformed nucleus [28].

The regularly-spaced energy spectra in Pd and Cd might naively be interpreted as a collective vibrational motion. At present it is not clear how nuclear vibration can be described properly from a microscopic shell model perspective. On the other hand, it is suggested that the apparent collectivity in the spectrum of Pd may have a different origin than that resulting from a vibration or rotational motion usually attached to nuclear collective phenomena [11, 12]. Since there is no evidence for shell interferences in the spectra of Pd isotopes, we will analyze other sources which control the structure of those spectra, namely the different coupled pair modes. This can be done rather easily in this case where the shell is very dominant, by considering separately the various components of the interaction. We found that when the interaction is switched off, the corresponding spectrum is of seniority type. This underlines the importance of the interaction to induce collective spectra.

To probe the pair content in the many-fermion wave function one may evaluate the two-particle transfer amplitude or the average number of pairs or project the shell-model wave functions onto a pair coupled basis with the help of the two-particle coefficients of fractional parentage. In Refs. [11, 12, 29] we applied the two-particle coefficients of fractional parentage technique. Two sets of the orthonormal bases are constructed starting from the monopole and pairs. In Refs. [24, 30, 31] all possible combinations are considered within an non-orthogonal basis by applying the so-called multistep shell model. After projecting the yrast wave functions into a product of isoscalar pairs we found the most striking feature of this case: all low-lying yrast states are built mainly from spin-aligned pairs as . In contrast to the isovector pairing excitations, in the aligned isocalar pair state there is no pair breaking when the nucleus is excited from one state to higher lying states in the spectrum. Instead, angular momentum in Pd is determined by a new form of coupling [11]. The mode can be deemed as a collective pair coupling scheme which can be written as a coherent superposition of all isovector neutron and proton pairs occupying the shell in the form of . The dynamics of the system is determined by the active four hole pairs aligned differently according to the total angular momentum of the system.

In a restricted single shell, the calculations of the average pair number can be much simplified with the help of two-particle coefficients of fractional parentage as

(1) |

and

(2) | |||||

where is the number of particles (holes) of the system and are the expansion amplitudes of the wave function. The Greek letters denote the basis states and the summation runs over all possible states.

For systems with four pairs the total number of interacting pairs is

(3) |

For a low-lying yrast state in Pd which has total isospin , the total number of isoscalar pairs is

(4) |

If isospin symmetry is assumed, the numbers of isovector neutron-neutron, proton-proton and pairs are the same and the total number of pairs is

(5) |

The results for the isoscalar pairs thus obtained in the space are shown in the left panel of Fig. 3. One sees that all low-lying yrast states are built mainly from spin-aligned pairs. In contrast to the isovector pairing excitations, in the aligned isoscalar pair state there is no pair breaking when the nucleus is excited from one state to higher lying states in the spectrum. Instead, the angular momentum of excited yrast states in Pd is generated by the rearrangement of the angular momentum vectors of the aligned pairs while the isoscalar pair character itself is preserved. For the ground state the four pairs are maximally aligned in opposite directions as allowed by the Pauli principle. When exciting the nucleus from one yrast state to another, the dynamics of the system is determined by the active four hole pairs aligned differently according to the total angular momentum of the system. It should be mentioned that the microscopic origin of the equidistant pattern generated by the aligned pairs remain unclear at present. From a simple semiclassical point of view, one may argue that the corresponding energies vary approximately linearly with for small total angular momenta, inducing similar energy spacings between consecutive levels.

To gain deeper physical insight into the structure of Pd we also calculated the numbers of isovector pairs which are plotted in the right panel of Fig. 3. It is seen that already in the ground state we have much more pairs with than the normal pair. In particular, the dominating component is the pair which is maximally aligned in the isovector channel. This is due to the large overlap between states generated by the spin-aligned pairs and those generated by the isovector pairs. This phenomenon is not seen in systems with two pairs where the contributions from the isovector aligned pair is practically zero for low-lying yrast states [24]. It should be emphasized that the dominating component in the wave functions of low-lying yrast states in Pd is still the spin-aligned pair coupling. But it may be interesting to clarify the role played by the isovector aligned pair in systems with more than two pairs. Work on this direction is underway.

The four pairs in Pd can couple in various ways. With the help of two-particle cfp one may express the wave function in terms of . It is thus found that, among the various aligned np pair configurations, the dominating components can be well represented by a single configuration . In the shell, this configuration is calculated to occupy around 66% of the ground state wave function of Pd, i.e., with amplitude [12]. Also it should be mentioned that the term is not the generator for the full aligned np coupling. It only generates the stretch configuration [13] shown above. The maximal state corresponds to a pure stretch configuration. On the other hand, by rewriting the wave function of Pd as a product of two group with two pairs (i.e., Cd each) within an non-orthornormal basis it is thus found the leading component is coupling Cd(gs)Cd(gs), as can also be seen from Fig. 4. This is consistent with the weak coupling calculations for light nuclei [16].

Usually the vibrational spectrum is characterized by collective E2 transitions between states differing by one phonon, where the corresponding transition strengths increase linearly as a function of the spin of the initial state. One of the most important criteria to decide whether a spectrum corresponds to the one of a vibrator is that there should be a nearly-degenerate two-phonon triplet with collective E2 transitions to the one-phonon state . In Fig. 5 we plotted the low-lying level scheme of Pd predicted by shell model calculations with the interaction of Ref. [21]. It is seen that there is indeed a triplet of states in the calculated spectrum which are nearly degenerate and lie at twice the energy of the state . The vibrational model predicts that the E2 transitions from the two-phonon states to the state should all have the same strength and its value should be twice that of the strength. This prediction differs very much from the calculated values for the aligned coupling scheme shown in the Figure. In particular, the strength of the transition is one order of magnitude smaller than the predicted value for a vibrator. This may be due to the fact that the calculated second state contain large contributions from shells (in particular the shell) other than the shell. That is, this state does not correspond to the spin-aligned coupling scheme proposed in this work. Indeed, this state cannot be reproduced in calculations within the shell.

The three yrast states in Fig. 5 are mainly composed of the spin-aligned pairs [12]. For example, the state is dominated by the configuration of with . The projection of this state on the stretch configuration is . It should be mentioned that the second state in Pd is also dominated by the spin-aligned pair coupling. In this state the largest two components are with and . This is in contrast with the coupling of pairs where only one state can be generated from the monopole pairs irrespective of the number of pairs involved. An interesting question would be how many states can we construct from the aligned pairs. A detailed analysis will be done elsewhere.

The proposed spin-aligned coupling may also shed some new light on the structure of odd-odd nuclei. Here we take the nucleus Ag as an example. It has three hole pairs in the Sn core. The calculated spectra of Ag in different model spaces are plotted in Fig. 6. The ground state is calculated to be and and is dominated by the coupling of two aligned pair and a normal isovector pair. The lowest state is calculated to be a state with excitation energy MeV. This state is dominated by the aligned pair coupling of with in restricted calculations performed within the shell. This component decreases to for the first state, which is otherwise dominated by the coupling . Again the wave functions of these states are mixtures of many components if we express them in the normal proton-proton and neutron-neutron coupling scheme.

In the right panel of Fig. 6 we evaluated the wave function of the state in Ag in the shell with a schematic Hamiltonian containing two interaction terms with and . It is thus found that the wave function shows a pure configuration of Cd(gs) for the calculation with a term only, while the stretch configuration Cd() gradually takes over by enhancing the strength of the aligned pair interaction. Similar calculations were also done for the state. For the wave function is characterized by the pure configuration Cd(gs) which is calculated to be the dominated component over a large range of . The contribution from the stretch configuration Cd() is also enhanced by enlarging the interaction .

To gain deeper insight into the properties of the aligned pair structure and the regions of the nuclear chart where this exotic mode can be observed, we also performed calculations for the , mass region. It is noted that, when the calculations are restricted to the shell only, both the nuclei Ti and Cr exhibit an equally-spaced pattern similar to the one obtained with the shell , as can be seen in Fig. 7. However, the aligned np coupling is not manifested in the spectra of the shell since the proximity of the shell and the strong quadrupole interaction thus developed leads to the mixing of shell model configurations that break the spin-aligned pair structure. As a result of this a combination of pairing and quadrupole interaction forms a more favorable description and a deformed mean field is generated. To explore further the role played by the aligned pair in this shell, we calculated the yrast spectra of Cr with different strengths for the interaction. It is thus found that a transition from rotational-like spectrum to vibrational-like spectrum occurs by enhancing the strength of the interaction element. On the contrary, our calculations show that in the mass 90-100 region and the shell the quadrupole interaction with the level is not strong enough to scatter nucleons appreciably across the energy gap associated with the magic numbers . Work underway is to explore in a more quantitative way the influence of deformation on the aligned pair coupling.

Another ongoing work is to generalize the aligned pair coupling to systems with more than one shell. This generalization may not be straightforward within the shell model framework due to the fact that the corresponding aligned pairs can carry different angular momenta. One possibility to overcome this drawback is through introducing as building blocks four-body quartets which are composed of aligned pairs [34].

## Acknowledgments

This work has been supported by the Swedish Research Council (VR) under grant Nos. 623-2009-7340 and 621-2010-4723. CQ thanks Prof. Honma for sending him the interaction matrix elements of the model space.

## References

## References

- [1] Bohr A 1976 Rev. Mod. Phys. 48 365.
- [2] Bohr A and Mottelson B R 1980 Phys. Scr. 22 468.
- [3] Rowe D J, Bahri C, Wijesundera 1998 Phys. Rev. Lett. 80 4394.
- [4] Rosensteel G and Rowe D J 2007 Nucl. Phys. A 797 94.
- [5] Goodman A L 1979 Adv. Nucl. Phys. 11 263.
- [6] Satuła W and Wyss R 1997 Phys. Lett. B 393 1.
- [7] Sheikh J A and Wyss R 2000 Phys. Rev. C 62 051302(R).
- [8] Dukelsky J, Gueorguiev V G, Van Isacker P, Dimitrova S, Errea B, Lerma S 2006 Phys. Rev. Lett. 96 072503.
- [9] Lerma S, Errea B, Dukelsky J, and Satuła W 2007 Phys. Rev. Lett. 99 032501.
- [10] Sandulescu N, Errea B, Dukelsky J 2009 Phys. Rev. C 80 044335.
- [11] Cederwall B et al. 2011 Nature 469 68.
- [12] Qi C, Blomqvist J, Bäck T, Cederwall B, Johnson A, Liotta R J, and Wyss R 2011 Phys. Rev. C 84 021301(R).
- [13] Danos M and Gillet V 1967 Phys. Rev. 161 1034.
- [14] Danos M and Gillet V 1966 Phys. Rev. Lett. 17 703.
- [15] Bhatt K H and McGrory J B 1971 Phys. Rev. C 3 2293.
- [16] Wong S K M and Zuker A P 1971 Phys. Lett. 36B 437.
- [17] Chen H T, Feng D H and Wu C L 1992 Phys. Rev. Lett. 69 418.
- [18] Garnsworthy A B et al. 2008 Phys. Lett. B 660 326.
- [19] Marginean N et al. 2001 Phys. Rev. C 63 031303(R).
- [20] NuDat 2.5. http://www.nndc.bnl.gov/nudat2/.
- [21] Honma M, Otsuka T, Mizusaki T and Hjorth-Jensen M 2009 Phys. Rev. C 80 064323.
- [22] Johnstone I P and Skouras L D 2001 Eur. Phys. J. A 11 125.
- [23] J. P. Schiffer and W. W. True, Rev. Mod. Phys. 48, 191 (1976).
- [24] Qi C 2010 Phys. Rev. C 81 034318.
- [25] Qi C and Xu F R 2008 Chin. Phys. C 32 (S2) 112.
- [26] Talmi I 2011 AIP Conf. Proc. 1355 121.
- [27] Talmi I 1993 Simple Models of Complex Nuclei (Harwood Academic Publishers, Chur, Switzerland).
- [28] Juodagalvis A 2000 arXiv:nucl-th/0004050.
- [29] Qi C 2011 Phys. Rev. C 83 014307.
- [30] Qi C, Wang X B, Xu Z X, Liotta R J, Wyss R, and Xu F R 2010 Phys. Rev. C 82 014304.
- [31] Xu Z X, Qi C, Blomqvist J, Liotta R J, Wyss R 2011 arXiv:1108.0269.
- [32] Poves A, Zuker A P 1981 Phys. Rep. 70 235
- [33] Escuderos A, Zamick L, Bayman B F 2005 arXiv:nucl-th/0506050
- [34] Shah J A and Danos M 1969 Phys. Rev. 183 899.