Abstract

In rare cases, the removal of a single proton (Z) or neutron (N) from an atomic nucleus leads to a dramatic shape change. These instances are crucial for understanding the components of the nuclear interactions that drive deformation. The mercury isotopes (Z = 80) are a striking example1,2: their close neighbours, the lead isotopes (Z = 82), are spherical and steadily shrink with decreasing N. The even-mass (A = N + Z) mercury isotopes follow this trend. The odd-mass mercury isotopes 181,183,185Hg, however, exhibit noticeably larger charge radii. Due to the experimental difficulties of probing extremely neutron-deficient systems, and the computational complexity of modelling such heavy nuclides, the microscopic origin of this unique shape staggering has remained unclear. Here, by applying resonance ionization spectroscopy, mass spectrometry and nuclear spectroscopy as far as 177Hg, we determine 181Hg as the shape-staggering endpoint. By combining our experimental measurements with Monte Carlo shell model calculations, we conclude that this phenomenon results from the interplay between monopole and quadrupole interactions driving a quantum phase transition, for which we identify the participating orbitals. Although shape staggering in the mercury isotopes is a unique and localized feature in the nuclear chart, it nicely illustrates the concurrence of single-particle and collective degrees of freedom at play in atomic nuclei.

Main

Atomic nuclei, comprising protons and neutrons, exhibit a rich array of quantum phenomena. These complex many-body systems obey the Pauli exclusion principle which dictates a nucleonic shell-like structure, akin to Bohr’s model of electrons in an atom. In the vicinity of closed shells, at the magic numbers of Z, N = 8, 20, 28, 50, 82 and N = 126, the nuclear wavefunction is dominated by the last few particles (or holes) and excitations thereof. In contrast to this single-particle nature, collective behaviour appears away from the closed shells, as increased nucleon–nucleon correlations drive the minimum-energy configuration of the nucleus to deformation. Consequently, the ground states of most isotopes in the nuclear chart are non-spherical. Most commonly they are prolate (rugby-ball) shaped, although different shapes, corresponding to alternative nucleon configurations, can coexist within the same nucleus3,4. It remains a challenge to pin down the full picture of the underlying microscopic origin of this phenomenon.

Optical spectroscopy is able to measure subtle shifts in the energy of the atomic electron levels, arising from changes in the charge distribution of the nucleus5. Along the isotopic chain of a given element, this effect is known as the isotope shift. From this, the change in mean-square charge radius, δ〈r2〉, can be extracted in a nuclear-model-independent way. Similarly, the hyperfine splitting of the electronic levels gives direct access to the nuclear properties: spin (I), magnetic dipole (μ) and electric quadrupole (Q) moments. Such measurements are therefore a sensitive and direct probe of the valence particle configuration and changes in nuclear size or deformation as a result of the addition or removal, and consequential redistribution, of nucleons.

The radioactive isotopes in the lead region have been the subject of a variety of optical spectroscopy studies for several decades. An intensified interest in this region was sparked by the study of the mercury isotopic chain, in which a sudden and unprecedented increase in charge radius was observed for 185Hg, 183Hg and 181Hg (refs 1,2). For the heavier mercury isotopes the changes in charge radii mirror those of lead6: steadily shrinking with decreasing N. This seminal discovery of shape staggering between odd and even neutron-deficient mercury isotopes is unparalleled elsewhere in the nuclear chart and was key to establishing the idea of shape coexistence at low excitation energy4,7. A plethora of studies on the excited states of these nuclei8,9 provided a further substantial insight into shape coexistence, complementing the laser spectroscopy studies of ground and isomeric states. However, to acquire a full understanding of this spectacular occurence requires its precise localization by probing even more neutron-deficient systems, which were previously experimentally inaccessible. Likewise, theoretical progress has been thwarted by the enormous computational requirements of a fully microscopic, many-body calculation of such heavy systems.

In this Letter we report breakthroughs on both fronts that now provide explanations of the underlying mechanism and localized nature of this shape staggering: the combination of state-of-the-art radioisotope production and detection techniques (see Fig. 1a) at the CERN-ISOLDE radioactive ion beam facility10, extending laser spectroscopy measurements to four lighter mercury isotopes (177–180Hg); and the exploitation of recent advances in computational physics to perform configuration interaction (CI) Monte Carlo shell model (MCSM)11 calculations with the largest model spaces to date.

Fig. 1: An overview of the in-source resonance ionization spectroscopy study of radiogenic mercury isotopes.
Fig. 1

a, Mercury isotopes are produced by proton-induced nuclear reactions in a molten lead target. The vapour effuses into the anode volume of the VADLIS ion source23, where the atoms are ionized using a three-step resonance photo-ionization scheme (inset). The ions are extracted as a mono-energetic beam at 30 keV. The isotope of interest is selected using the general-purpose mass separator (GPS) and directed towards the most appropriate of the three detection systems shown (see Methods). b, By scanning the laser wavelength of the spectroscopic transition (in this case the first step), the isotope shift (IS) and hyperfine structure (HFS) are examined. The isotope shifts are used to calculate the changes in mean-square charge radii δ〈r2〉 with respect to A = N + Z = 198 along the isotopic chain. c, The results of this study appear as filled red circles (ground states, gs) or open red circles (isomeric states, is). 177−180Hg are new measurements, whereas 181−185Hg were re-measured and the data points overlap with those of the literature values (blue circles), as can also be seen by the close agreement between values in Table 1. The error bars correspond to the standard deviation of measurements. Additional scaling uncertainties (not shown) arise from the indeterminacy of the F factor (7%; see ref. 19) and the specific mass shift, MSMS. These are provided in Table 1. The additional continuous black line illustrates the previously measured quasi-spherical trend of the lead nuclei6. Sketched insets, representative of the shapes of 190Hg and 181Hg with a deformation parameter 〈β221/2 = 0.174 and 0.313 respectively, are provided.

Ground-state and isomer charge radii and magnetic moments were studied by performing resonance ionization spectroscopy on the mercury isotopes with unprecedented sensitivity, reaching as far as 177Hg, an isotope with a half-life of only 127 ms and a production rate of just a few ions per minute. The new experimental scheme is illustrated in Fig. 1a, with the recorded optical spectra shown in Fig. 1b and resulting charge-radii data in Fig. 1c. The isotope shifts measured relative to 198Hg and the deduced changes in mean-square charge radii and moments for 177−185Hg are presented in Table 1. A complete description of the data analysis and fitting can be found in the doctoral theses of T. Day Goodacre12 and S. Sels13. The close agreement between the values extracted from this work and those of literature is a convincing validation of our technique and data treatment.

Table 1 Summary of resulting mean-square charge differences (δ〈r2A−198) and nuclear moments (μ, Q) and their comparison to literature. δ〈r2〉 (lit.) values were recalculated from the measured IS19 with the same F and MSMS factors as in the present work

The changes in mean-square charge radii of mercury isotopes combined with those of the lead isotopes6 are shown relative to A = 198 in Fig. 1c. In addition to confirming the earlier results, these new data firmly prove that the dramatic shape staggering is a localized phenomenon and that the odd-mass mercury isotopes return to sphericity at A = 179 (N = 99).

To pinpoint the microscopic origin of this observation, we performed large-scale numerical simulations for the quantum many-body problem using a MCSM method. Heavy nuclei such as the mercury isotopes are beyond the limit of conventional CI calculations for protons and neutrons interacting through nuclear forces. However, using the MCSM method and the most advanced computers has allowed us to reach this region for the first time, redefining the state of the art of CI calculations for atomic nuclei. Calculations were performed for the ground and the lowest excited states in 177−186Hg with spin and parity corresponding to the experimental ground-state values of the nuclei considered: 0+ for the even-mass isotopes, 1/2 for 181,183,185Hg and 7/2 for 177,179Hg. Also the 13/2+ long-lived isomer in 185Hg was examined. The MCSM provides the eigen wavefunction from which the magnetic dipole and electric quadrupole moments, and the shape parameters (β2, γ) are calculated14. In turn, the shape parameters are used to obtain the mean-square charge radius (see Methods). For all these states, the changes in mean-square charge radii relative to the ground state of 186Hg are presented as shaded boxes in Fig. 2a. The height of the shaded box is related to the spread of the quantum fluctuations of the MCSM eigenstates, examples of which are shown by the distribution of β2 values in Fig. 2d (see Methods for more details). Figure 2 shows that for every mercury isotope, only one state can be identified for which the calculated δ〈r2〉 is in agreement with experiment. For the odd-mass nuclei this identification is confirmed by the agreement between the calculated and measured magnetic moments, as shown in Fig. 2b. Furthermore, with the exception of 181Hg, for which the calculated energy difference between \(1/2_3^-\) and \(1/2_1^-\) states is only 218 keV, and in spite of the limited number of basis vectors used, the selected MCSM states indeed correspond to the ground states in the calculations. The remarkable agreement with the experimental data that has been achieved reinforces our confidence in the ability of this MCSM method to reveal the discrete changes in the nuclear configuration that drive shape coexistence in this region. We therefore gain an insight into the underlying mechanism responsible for the sudden appearance and disappearance of the uniquely pronounced shape staggering in the mercury isotopes.

Fig. 2: A comparison of the experimental results with the MCSM calculations for the mercury isotopes studied in this work.
Fig. 2

a, Plot of δ〈r2〉 relative to that of the ground state of 186Hg. Red points are experimental data from this experiment. They include the combined statistical (standard deviation) and systematic uncertainties quoted in Table 1. Blue points refer to literature values from ref. 19. The shaded boxes indicate radii corresponding to the MCSM eigenstates labelled by their respective spin J, parity π and energetic ordering i as \(J_i^\pi\). The grey areas show MCSM eigenstates for which the calculated magnetic moment differs from the measured value. b, Comparison of the calculated and experimental magnetic moments for different states in the odd-mass mercury isotopes. c, The occupation numbers of the neutron i13/2 orbit and the proton h9/2 orbit for the states indicated by the blue connected areas in a (these are the experimentally observed ground states). The deviation of the three strongly prolate deformed states at A = 181, 183, 185 from the general occupancy trend is evident. d, So-called T-plot14,24 examples for two different states in 185,186Hg, with large and small deformations, respectively. The corresponding β2 and γ shape parameters of the main contributing MCSM basis vectors are denoted by orange circles (see text and Methods).

The MCSM enables us to examine the microscopic composition of each MCSM state in terms of the occupancy of the proton and neutron orbitals (see Fig. 2c). The most striking differences between the deformed 1/2 states in 181,183,185Hg and the other near-spherical states are found in the nucleon-occupancy of two orbitals: the proton 1h9/2 situated above the Z = 82 closed shell and the neutron 1i13/2 midshell between N = 82 and N = 126. The strongly deformed 1/2 states of 181,183,185Hg exhibit large and constant values (~8) of the neutron 1i13/2 occupation number, as well as a sizeable promotion of two to three protons across the Z = 82 magic shell gap to the 1h9/2 orbit.

This abrupt and significant reconfiguration of the nucleons originates not only from the quadrupole component of the nucleon–nucleon (NN) interaction, known to be responsible for inducing deformation in atomic nuclei, but also in the monopole component. The strong attractive nature of the latter, specifically between the proton 1h9/2 orbital and neutron 1i13/2 orbital, results in an additional lowering of the binding energy14. If this energy gain, combined with that of the quadrupole deformation, exceeds the energy needed to create particle–hole excitations then the deformed state becomes the ground state.

It is thus the combined action of the monopole interaction, the effect of which depends linearly on the orbital occupancy numbers, and the quadrupole interaction, which follows a quadratic dependence with a maximum when an orbital is half-filled (that is seven neutrons in the 1i13/2 orbital), that delineates the deformed region for the mercury isotopic chain between N = 101 and N = 105. For even-N mercury isotopes, the pairing correlation that exists for the spherical shape produces sufficient binding energy because of the high-level density, whereas this is suppressed in odd-N isotopes due to blocking of the unpaired neutron. The strongly deformed state, assisted by the combined monopole and quadrupole effect, therefore becomes the ground state. Thus, the observed shape staggering is due to a subtle competition between these two shapes, which are different in terms of their many-body configuration.

The shape staggering effect manifests characteristic features of a quantum phase transition15,16,17: in a given nucleus, different phases—a near spherical and a strongly deformed nuclear shape—appear at almost the same energy without mixing. By making small changes in the control parameter, which in this case is the neutron number, the system alternates between the two phases. In the case of the mercury chain, this observation, which resembles a critical phenomenon in phase transitions, happens six times. This unique feature is now quantitatively understood through the MCSM calculations, highlighting the importance of the simultaneous multiple excitations to the proton 1h9/2 and neutron 1i13/2 orbitals14. In this picture, because of the major role of the neutron 1i13/2 orbital in driving the large quadrupole deformation, this effect can dominate only close to neutron number N = 103. By delineating the region of shape staggering, our new data provide the neccessary information to support this picture.

Extending the isotope shift and hyperfine structure measurements to the other extremely neutron-deficient nuclei below midshell at N = 104, either side of the Z = 82 shell closure is important. This will enable us to check the dependence of the deformation evolution on the proton number, and particularly on the proton 1h9/2 orbital occupancy. It will then be possible to understand whether the same mechanism is responsible for shape changes in other isotopic chains in this region.

The MCSM calculation is shown, by this work, to be applicable to spectroscopic studies on heavy nuclei. These nuclei are located at the current feasibility limit, and thereby the calculation has been done for selected states, and only energies and moments are obtained. Thanks to rapid developments in supercomputing, more states will soon be calculated systematically, and dynamical properties such as band structure and spectroscopic factors will be clarified. This is in perfect accordance, for example, with the ongoing experimental programmes at CERN/ISOLDE on Coulomb excitation and nucleon transfer reactions, making use of post-accelerated radioactive ion beams18.

Methods

Mercury isotope production

The experiment was performed at the CERN-ISOLDE isotope separator facility10. Neutron-deficient mercury isotopes were produced by proton-induced spallation of lead nuclei: a molten lead target was bombarded with protons from the CERN Proton Synchroton booster at an energy of 1.4 GeV. The proton beam intensity (1 × 1013 protons per pulse, up to 1 μA averaged current) and bunched proton extraction were optimized to enhance the release of short-lived isotopes from the liquid target whilst reducing the likelihood of a mechanical failure due to shockwaves generated by the proton impact25,26. A temperature-controlled spiral chimney enables effusion of the mercury vapour towards the ion source cavity whilst ensuring the required suppression, by condensation, of less volatile species such as lead. The mercury atoms effuse into the anode cavity of a forced electron beam ion arc discharge (FEBIAD)-type ion source, referred to as the VADLIS (Versatile Arc Discharge and Laser Ion Source)23. For this experiment the laser beams from the Resonance Ionization Laser Ion Source (RILIS)27 laboratory were directed into the FEBIAD anode cavity through the 1.5 mm ion extraction aperture. The lasers were tuned to the three-step resonance ionization scheme for mercury (Fig. 1a inset)28, resulting in laser-ionization of mercury only. For the first time during on-line operation, the ion source was operated in the newly established RILIS mode, whereby the anode voltage is reduced to several volts, while the cathode heating and ion source magnetic field strength are optimized for laser-ion survival and extraction. In this case, no electron impact ionization occurs, and the laser-ionized Hg+ beam purity is maximized. The ion source efficiency remains similar to that of standard FEBIAD operation with electron-impact ionization (estimated to be several per cent). Mercury ions leaving the anode exit aperture are subject to the 30 kV potential difference between the ion source aperture and the grounded extraction electrode. The resulting mono-energetic beam of mercury ions was then passed through a magnetic dipole mass separator, which has sufficient resolution for the selection of the atomic mass of interest for transmission to the detection system, but is not capable of separating isobars.

Laser spectroscopy and signal identification

To extend our reach beyond the range of previously studied mercury isotopes, it was necessary to use the most sensitive laser spectroscopy method available at ISOLDE: in-source resonance ionization spectroscopy. Laser resonance ionization is commonly used for radioactive ion beam production at many facilities worldwide29,30 and the unmatched sensitivity achieved by optimizing this method for laser spectroscopy during the initial ion creation is well recognized5. Wavelength-tuning of one of the lasers used in the resonance ionization scheme directly influences the ionization efficiency of the element of interest. For this work the 254 nm first-step transition (6s2 1S0 → 6d6p 3P1°) of the ionization scheme was used for spectroscopy since its sensitivity to nuclear variations results in a well-resolved hyperfine structure, despite the high-temperature (approximately 1,800 °C) of the ion source cavity (where Doppler broadening of the atomic spectral lines is dominant). The 254 nm light required was produced by third-harmonic generation from the output of a Ti:Sapphire laser, operating in the dual etalon scanning mode (fundamental linewidth of 0.8 GHz)31. While operating the ion source in RILIS-mode, this laser was scanned in a stepwise manner and at each frequency step the ion rate was recorded using the most suitable of the three detection methods available. Depending on the intensity, purity, lifetime or decay mode of the beam at a chosen mass, the ion beam was directed to one of the three detection systems depicted in Fig. 1a: the ISOLDE Faraday cup, for ion current measurements above 100 fA; the ISOLTRAP MR-ToF MS, for isobar-separated ion counting of longer-lived isotopes with a resolving power of MM ≈ 300,000 (refs 32,33); or the Windmill decay spectroscopy set-up (for efficient detection of alpha-decaying isotopes). Laser scans were obtained for all 177−185Hg ground states. The isotope shifts were determined relative to 198Hg. A total of 17 198Hg reference scans were recorded periodically during the experiment.

MCSM calculations

The MCSM calculation is one of the most advanced computational methods that can be applied for nuclear many-body systems. This work represents the largest ever MCSM calculations, performed on massively parallel supercomputers, including the K computer in Kobe, Japan. Exploiting the advantages of quantum Monte Carlo, variational and matrix-diagonalization methods, this approach circumvents the diagonalization of a >2 × 1042-dimensional Hamiltonian matrix. Using the doubly-magic 132Sn nucleus as an inert core, 30 protons and up to 24 neutrons were left to actively interact in an exceptionally large model space as compared to conventional CI calculations. Single-particle energies were set to be consistent with single-particle properties of 132Sn and 208Pb, with smooth changes as functions of Z and N. All nucleons interact through effective NN interactions adopted from the frequently used ones34,35. The Hamiltonian was thus fixed and kept throughout this study. The model spaces in which the nucleons interact are 11 proton orbits from 1g7/2 up to 1i13/2 and 13 neutron orbits from 1h9/2 up to 1j15/2. Calculations were performed using effective charges for protons and neutrons, with their actual values being 1.6e and 0.6e, respectively, and a spin quenching factor of 0.9. The MCSM eigenstate is represented as a superposition of MCSM basis vectors with the appropriate projection onto spin and parity. Each MCSM basis vector is a Slater determinant formed by mixed single-particle states, where the mixing amplitudes are optimized by quantum Monte Carlo and variational methods. This Slater determinant has intrinsic quadrupole moments, which can be expressed in terms of a set of β2 and γ deformation parameters. Using the effective charges and spin quenching factor, we reproduce the electric quadrupole moments of 177,179Hg and the magnetic dipole moments of the odd-mass mercury isotopes (see Fig. 2b). The combined effect of the monopole interaction, which depends linearly on the orbital occupancy numbers, and the quadrupole interaction, which contains a quadratic dependence with a maximum when an orbital is half-filled, causes the observed shape staggering. Specifically, the strong attractive monopole matrix element between proton h9/2 and neutron i13/2 orbitals (−0.35 MeV), compared to an average value of −0.2 MeV for the other orbitals considered, localizes the observed phenomena around N = 103 (ref. 14). This is due to the similarity in radial wavefunctions and the coherent sizeable effect of the tensor force35.

Using the effective charges, the quadrupole moments for each MCSM basis vector can be obtained. These can be converted into the standard ellipsoidal nuclear shape parameters β2 (deformation strength) and γ (deformation shape)36. One of the strengths of the MCSM is the ability to link the basis vectors onto the Potential Energy Surface (PES) deduced using the same NN interaction. The T-plot14,24 was introduced to indicate the individual MCSM basis vectors using β2 and γ as partial coordinates on the PES.

Figure 2d shows example T-plots for 185,186Hg. The importance of each MCSM basis vector is evaluated in terms of the probability amplitude in the eigenstate of interest, as shown by the size of the circle: larger circles represent major MCSM basis vectors, whereas smaller circles imply a less relevant contribution to this particular eigenstate. In these T-plots, clustering of the circles is observed for spherical (186Hg) and prolate shapes (185Hg).

To compare the δ〈r2〉 from the isotope shift measurements to the β2 deduced from the MCSM calculations, the following standard procedure was used:

$$\left\langle {r^2} \right\rangle = \left\langle {r^2} \right\rangle _{{\mathrm{DM}}}\left( {1 + \frac{5}{{4\pi }}\left\langle {\beta _2} \right\rangle ^2} \right)$$
(1)
$$\delta \left\langle {r^2} \right\rangle ^{A - 186} = \left\langle {r^2} \right\rangle - \left\langle {r^2} \right\rangle ^{186}$$
(2)

where 〈r2DM refers to the droplet model mean square charge radius, for which the most-used parametrization of Berdichevsky and Tondeur37 is adopted. Following this procedure, the influence of γ is negligible.

The calculated δ〈r2〉, shown in Fig. 2a, are indicated by shaded boxes. The height of the box is determined by the distribution of the circles in the T-plot with respect to β2 and represents the spread of the quantum fluctuations of the MCSM eigenstates.

Data availability

All of the relevant data that support the findings of this study are available from the corresponding author upon reasonable request.

Additional information

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Acknowledgements

This work has received funding through the following channels: the Max-Planck-Society, IMPRS-PTFS; BMBF (German Federal Ministry for Education and Research) Nos. 05P12HGCI1 and 05P15HGCIA; STFC Grant Nos. ST/L005727, ST/M006433, ST/M006434, ST/L002868/1, ST/L005794/1; Slovak Research and Development Agency, contract No. APVV-14-0524; European Unions Seventh Framework Programme for Research and Technological Development under Grant Agreements 267194 (COFUND) and 289191 (LA3NET). FWO-Vlaanderen (Belgium), by GOA/2015/010 (BOF KU Leuven); the Inter-university Attraction Poles Programme initiated by the Belgian Science Policy Office (BriX network P7/12), by the European Commission within the Seventh Framework Programme through I3-ENSAR (contract no. RII3-CT-2010-262010) and by a grant from the European Research Council (ERC-2011-AdG-291561-HELIOS). S.S acknowledges the Agency for Innovation by Science and Technology in Flanders (IWT). L.P.G acknowledges FWO-Vlaanderen (Belgium) as an FWO Pegasus Marie Curie Fellow. A.W and K.Z acknowledge the Wolfgang-Gentner scholarship and the BMBF (German Federal Ministry for Education and Research) no. 05P12ODCIA. This work was supported by JSPS and FWO under the Japan-Belgium Research Cooperative Program. The MCSM calculations were performed on the K computer at RIKEN AICS (hp160211, hp170230). This work was also supported in part by Priority Issue on Post-K computer (Elucidation of the Fundamental Laws and Evolution of the Universe) from MEXT and JICFuS. J.D. and A.P. acknowledge partial support from the STFC grant No. ST/P003885/1. The density functional theory calculations were performed using the DiRAC Data Analytic system at the University of Cambridge, operated by the University of Cambridge High Performance Computing Service on behalf of the STFC DiRAC HPC Facility (www.dirac.ac.uk). This equipment was funded by BIS National E-infrastructure capital grant (ST/K001590/1), STFC capital grants ST/H008861/1 and ST/H00887X/1, and STFC DiRAC Operations grant ST/K00333X/1. DiRAC is part of the National e-Infrastructure.

Author information

Author notes

  1. These authors contributed equally: T. Day Goodacre, S. Sels.

Affiliations

  1. CERN, Geneva, Switzerland

    • B. A. Marsh
    • , T. Day Goodacre
    • , V. N. Fedosseev
    • , K. M. Lynch
    • , R. E. Rossel
    • , S. Rothe
    •  & M. Veinhard
  2. School of Physics & Astronomy, The University of Manchester, Manchester, UK

    • T. Day Goodacre
    • , N. A. Althubiti
    • , J. Billowes
    • , T. E. Cocolios
    • , G. J. Farooq-Smith
    • , K. T. Flanagan
    •  & S. Rothe
  3. KU Leuven, Instituut voor Kern- en Stralingsfysica, Leuven, Belgium

    • S. Sels
    • , T. E. Cocolios
    • , G. J. Farooq-Smith
    • , L. P. Gaffney
    • , L. Ghys
    • , M. Huyse
    • , Y. Martinez Palenzuela
    • , T. Otsuka
    • , C. Van Beveren
    • , P. Van Duppen
    • , E. Verstraelen
    •  & A. Zadvornaya
  4. Center for Nuclear Study, University of Tokyo, Tokyo, Japan

    • Y. Tsunoda
    •  & T. Otsuka
  5. Department of Nuclear Physics and Biophysics, Comenius University in Bratislava, Bratislava, Slovakia

    • B. Andel
  6. Department of Physics, University of York, York, UK

    • A. N. Andreyev
    • , J. G. Cubiss
    • , J. Dobaczewski
    •  & A. Pastore
  7. Advanced Science Research Center, Japan Atomic Energy Agency (JAEA), Tokai-mura, Japan

    • A. N. Andreyev
  8. Max-Planck-Institut für Kernphysik, Heidelberg, Germany

    • D. Atanasov
    • , K. Blaum
    • , S. Kreim
    • , V. Manea
    •  & R. N. Wolf
  9. Petersburg Nuclear Physics Institute (PNPI), NRC Kurchatov Institute, Gatchina, Russian Federation

    • A. E. Barzakh
    • , D. V. Fedorov
    • , P. L. Molkanov
    •  & M. D. Seliverstov
  10. School of Engineering & Computing, University of the West of Scotland, Paisley, UK

    • L. P. Gaffney
    •  & P. Spagnoletti
  11. CSNSM-IN2P3-CNRS, Universite Paris-Sud, Orsay, France

    • D. Lunney
  12. Department of Physics, University of Tokyo, Tokyo, Japan

    • T. Otsuka
  13. RIKEN Nishina Center, Wako, Japan

    • T. Otsuka
    •  & M. Rosenbusch
  14. National Superconducting Cyclotron Laboratory, Michigan State University, East Lansing, MI, USA

    • T. Otsuka
  15. Institut für Physik, Universität Greifswald, Greifswald, Germany

    • M. Rosenbusch
    • , L. Schweikhard
    •  & F. Wienholtz
  16. Technische Universität Dresden, Dresden, Germany

    • A. Welker
    •  & K. Zuber
  17. Johannes Gutenberg Universität, Mainz, Germany

    • K. Wendt

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Contributions

A.N.A, A.E.B, T.D.G, D.V.F, V.N.F, L.P.G, M.H, B.A.M, M.D.S. and P.V.D. conceived the experiment and prepared the proposal; T.D.G, D.V.F, V.N.F, B.A.M, Y.M.P, P.L.M, R.E.R, S.R. and M.V. carried out laser ionization scheme and/or ion source developments; A.N.A, K.B, T.E.C, V.N.F, M.H, S.K, B.A.M, L.S, P.V.D. and K.Z. supervised the participants; B.A, N.A.A, D.A, A.E.B, J.B, T.E.C, J.G.C, T.D.G, G.J.F.-S., D.V.F, V.N.F, K.T.F, L.P.G, L.G, M.H, K.M.L, V.M, B.A.M, Y.M.P, P.L.M, R.E.R, S.S, P.S, C.V.B, P.V.D, M.V, E.V, A.W, F.W. and A.Z. participated in data taking; T.O. and Y.T. performed MCSM calculations; J.D. and A.P. performed density functional theory calculations; A.E.B, T.D.G, D.V.F, B.A.M, P.L.M, R.E.R, S.R. and M.V. took part in laser set-up and operation; B.A, D.A, T.E.C, J.G.C, K.T.F, L.P.G, L.G, K.M.L, V.M, M.R, R.E.R, L.S, S.S, C.V.B, A.W, F.W. and R.N.W. set up and operated the detection and data acquisition systems; A.N.A, A.E.B, K.B, T.E.C, T.D.G, J.D, D.V.F, L.P.G, M.H, B.A.M, T.O, L.S, M.D.S, S.S, P.V.D, E.V. and K.W. contributed to the data analysis and interpretation; A.N.A, A.E.B, K.B, T.E.C, J.G.C, T.D.G, J.D, V.N.F, L.P.G, M.H, D.L, B.A.M, T.O, L.S, S.S, Y.T. and P.V.D. contributed to the manuscript preparation.

Competing interests

The authors declare no competing interests.

Corresponding author

Correspondence to B. A. Marsh.

About this article

Publication history

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DOI

https://doi.org/10.1038/s41567-018-0292-8

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