Astrophysical shocks are commonly revealed by the non-thermal emission of energetic electrons accelerated in situ1,2,3. Strong shocks are expected to accelerate particles to very high energies4,5,6; however, they require a source of particles with velocities fast enough to permit multiple shock crossings. While the resulting diffusive shock acceleration4 process can account for observations, the kinetic physics regulating the continuous injection of non-thermal particles is not well understood. Indeed, this injection problem is particularly acute for electrons, which rely on high-frequency plasma fluctuations to raise them above the thermal pool7,8. Here we show, using laboratory laser-produced shock experiments, that, in the presence of a strong magnetic field, significant electron pre-heating is achieved. We demonstrate that the key mechanism in producing these energetic electrons is through the generation of lower-hybrid turbulence via shock-reflected ions. Our experimental results are analogous to many astrophysical systems, including the interaction of a comet with the solar wind9, a setting where electron acceleration via lower-hybrid waves is possible.


Lower-hybrid waves occur in a variety of laboratory and space environments. They have been suggested to be an important electron-heating or energization mechanism in different magnetized plasma environments10,11,12. These waves propagate nearly transverse to the magnetic field lines and oscillate at a frequency between the ion gyro frequency and the electron gyro frequency. As a consequence, lower-hybrid waves with frequency ω and wavenumber k can be in simultaneous Cerenkov resonance, ω − kv = 0 (where v is the particle velocity), both with magnetized electrons propagating along the field lines and unmagnetized ions moving perpendicular to the field. The lower-hybrid waves have a high phase velocity along the field lines that resonate with the fast moving electrons as well as a low phase velocity across the field lines that resonate with the slow moving ions, allowing for energy transfer between the two species13 (see Methods for further details). This convenient property of lower-hybrid waves, as an efficient channel for the acceleration of electrons above the thermal background, is well known in the magnetically confined fusion community14, where it has been exploited with considerable efficacy in past experiments15,16. Although a different mechanism is favoured in toroidal field configurations, for highly oblique shocks, such as might be created in the solar wind9, supernova explosions11, or during the formation of galaxy clusters17, it is thought that the modified two-stream instability13, driven by reflected ions from the shock front, excites broad-band lower-hybrid modes. By comparing theoretical and numerical predictions with the experimental data on the modified two-stream instability, it may be possible to develop robust scaling relations to apply to the fusion-relevant parameters (see Methods for further discussion).

While electron acceleration by lower-hybrid waves in the Solar System has been inferred from satellite measurements9,18, laboratory experiments provide reproducible and controllable conditions that can be used not only as a means of supporting space observations, but also for validating multi-scale transport predictions from simulation codes19. Here we show the results from an experiment where a laser-produced plasma flow impacts on a magnetized sphere (see Fig. 1). This mimics, for example, the interaction of the solar-wind plasma with a comet9, an environment where excess X-ray generation by accelerated electrons has been observed. The scaling between the experiment and the comet interaction with the solar wind is determined by a set of parameters shown in Supplementary Table S1. While both lower-hybrid turbulence and charge exchange processes20 are possible explanations, our experimental results are compatible only with the former (see Supplementary Information).

Fig. 1: Illustration of a magnetized plasma–sphere interaction.
Fig. 1

a, Interaction of a comet with the solar wind. The relative motion between the incoming solar-wind ions and cometary pick-up ions, across the solar wind’s magnetic field, result in the formation of the modified two-stream instability (MTSI) that, in turn, can excite waves within the lower-hybrid frequency range. The lower-hybrid waves can transfer energy from the counter-streaming ions travelling perpendicular to the magnetic field into accelerating electrons parallel to the magnetic field, and so produce a suprathermal electron population. b, Schematic of the experimental set-up. A 1 kJ, 1.5 ns laser drive at 527 nm with a spot size of 200-μm-diameter is impacted onto a 50 μm PVDF (C2H2F2) foil target producing an expanding plasma jet from the back surface, as shown in the overlaid image of the 550–800 nm optical emission of the plasma. A 12-mm-diameter sphere is placed 15 mm from the target foil. The sphere is either a dipole magnetized neodymium sphere with an approximately 7 kG surface field or a non-magnetized soda glass sphere of the same diameter. Optical diagnostics (interferometry and SOP) have an approximately 25 mm field of view, 250 ps gate time, and look perpendicularly to the laser axis, similarly to the view above. An X-ray spectrometer spatially resolves along the laser axis with an RbAP crystal and spectrally resolves within the region from 630 to 770 eV.

The experiment was conducted at the LULI laser facility at École Polytechnique (France). Various diagnostics were implemented to probe the plasma before and after the interaction with the sphere (see Fig. 2 for details).

Fig. 2: Optical data and radiation-hydrodynamic simulations.
Fig. 2

a, SOP data for a non-magnetized sphere. The plasma emission in the optical band 550–800 nm along the flow axis is streaked in time for 500 ns. Vertical dashed lines indicate the position of the target and sphere; horizontal lines indicate the time at which the interferometry data and FLASH simulation snapshot were taken. The plasma reaches the sphere in 200 ns, indicating a flow velocity of 70 km s−1. b, Same as a but for a magnetized sphere. c, Transverse optical interferometry data taken at 300 ns for a non-magnetized sphere. The inferred electron density colour plot is overlaid (see Supplementary Information). d, Same as c but taken at 290 ns for a magnetized sphere. e, Snapshot of a radiation-hydrodynamic simulation with no external field after 400 ns, symmetric about the laser axis. Pseudocolour plots of electron temperature (top) and electron density (bottom) are shown. f, Same as e but with a constant 5 kG field perpendicular to the flow axis. Colour bars are the same for both e and f. g, Optical emission spectra of the plasma (dark blue solid line) at 300 ns, 12 mm from the target along the flow axis for the non-magnetized sphere case. Different spectra predicted by the code PrismSPECT (dashed lines) are overlaid and give a temperature best fit of 3 ± 1 eV (see Supplementary Information).

Streaked optical pyrometry (SOP) shows the optical plasma emission streaked in time. SOP indicates that the plasma travels at a velocity of 70 km s−1, implying the fluorine ions have a kinetic energy ~ 500 eV. The interferometry data show that, for the magnetized sphere, there is a bulk electron density of ~ 1017 cm−3 upstream of the shock, rising to 1018 cm−3 downstream of the shock. Optical spectroscopy data give a bulk plasma temperature of 3 ± 1 eV. The optical data indicate that the interaction of the plasma with the sphere is different for the magnetized and non-magnetized cases (see, for example, ref. 21). For the non-magnetized sphere, there is less pronounced plasma build-up in front of the sphere.

Near the axis of the flow, and close to the surface of the sphere, a shock with ~ 1 mm stand-off distance can be seen. In the magnetized case, the perpendicular field lines constrain the flow, making it more difficult for the plasma to fully flow around the sphere. Consequently, there is a larger pressure build-up in front of the sphere, generating a shock at ~ 2.5 mm stand-off position, larger than that of the non-magnetized case. Balancing the ram pressure of the plasma flow with that of the compressed magnetic field gives an estimation for the expected stand-off distance in the magnetized case of ~ 1 mm, similar to the experimental value.

To further understand the flow dynamics and its interaction with the sphere, two-dimensional radiation-magnetohydrodynamics (MHD) simulations were performed using the FLASH code (see Supplementary Information). The simulations agree qualitatively with experimental measurements, as shown in Fig. 2, while providing additional estimates of bulk plasma properties. The magnetic field carried by the ablated plasma is weak, and from the measured plasma parameters we infer the shock formed to be highly super-critical, with a fast magneto-sonic Mach number of 5.7 ± 0.2, necessitating a significant reflected ion component22. The electric field influencing the plasma near the shock can be estimated using the magnetic field and ion density calculated in FLASH (see Supplementary Information).

For the shock to reflect incoming ions, the cross-shock electric potential must exceed the kinetic energy of the incoming ions. FLASH simulations predict an electric field of ~ 70 MeV m−1 at a distance of 0.5 mm from the sphere at 300 ns, increasing as the simulation progresses. Assuming a shock thickness on the order of the electron skin-depth L ~ 10 μm results in a cross-shock potential approximately equal to 700 eV, sufficient to reflect incoming fluorine ions, with a kinetic energy of ~ 500 eV. These reflected ions produce the counter-streaming ion flow, which is necessary for generating lower-hybrid turbulence, an effect not captured in FLASH simulations.

We have probed the plasma emission in the soft X-ray range (630–770 eV) with an X-ray spectrometer that spatially resolved along the flow axis (see Supplementary Information). The integrated intensity of the observed fluorine X-ray line can then be plotted as a function of position along the flow axis (see Fig. 3). When the magnetized sphere is present, an excess in X-ray intensity is observed close to the sphere compared with the non-magnetized sphere. This excess in soft X-rays suggests that electrons of energies significantly greater than 3 eV must be present. As lower-hybrid turbulence requires the reflected ions to move perpendicularly to the field lines, we have also considered the case when the sphere was rotated to have the magnetic dipole moment aligned with the flow, mimicking a parallel field line configuration. In the latter configuration, we found no appreciable increase in X-ray intensity close to the sphere relative to the non-magnetized case.

Fig. 3: X-ray data.
Fig. 3

a, Integrated X-ray intensity of the fluorine He-α line as a function of position along the laser axis. Data for magnetized sphere shots (blue diamonds) have an increased intensity close to the sphere when compared with data for non-magnetized sphere shots (red circles). The error bars represent the standard deviation for each data point (see Supplementary Information for further details). b, Normalized X-ray signal, showing the fluorine He-α line for the non-magnetized (left) and magnetized (right) shots. For both cases, a white rectangle and an additional plot have been overlaid. The white rectangle indicates the region where the spatial lineouts were taken. The overlaid plots show the average spatially integrated spectral line shape within the white rectangle (that is, close to the sphere). The normalization for all the X-ray data has been chosen such that the peak intensity of the spectral line shape for the magnetized sphere in case b is set to unity.

To investigate further the lower-hybrid origin for the excess X-ray emission near the magnetized sphere, and the possible presence of a suprathermal electron population, we have performed 2D particle-in-cell (PIC) simulations of the plasma flow collision with the dipolar magnetic object (see Fig. 4) using the massively parallel, fully relativistic code OSIRIS (see Supplementary Information).

Fig. 4: OSIRIS PIC simulations.
Fig. 4

a, Injected ion density. b, Electron temperature. c, Wave spectrum. The wave spectrum is calculated by performing a Fourier transform on the ion density to gain information on the parallel and perpendicular k-numbers. The black dashed lines indicate modes that have a ratio in k-number consistent with the lower-hybrid dispersion relation for ions reflected horizontally off of the shock. The black dotted lines indicate modes that have a ratio in k-number consistent with the lower-hybrid dispersion relation for ions reflected on the flanks of the bow shock. All figures are taken at the same time of 6 ion cyclotron periods.

OSIRIS simulation results indicate, in agreement with our previous FLASH simulations, that as the plasma impacts the sphere (of typical size larger than the ion Larmor radius), a bow shock develops23. The counter-propagating ion flow is unstable and excites plasma waves in the lower-hybrid range ahead of the shock front (see Fig. 4). These waves are then amplified and break, resulting in a turbulent, compressed plasma region. In fact the ratio between the parallel (k||) and perpendicular (k) wavenumber of these modes is consistent with the idealized dispersion relation for lower-hybrid waves of \(\frac{{k}_{\parallel }}{{k}_{\perp }}\approx \sqrt{\frac{{m}_{\rm{e}}}{{m}_{\rm{i}}}}\)9, as highlighted in Fig. 4 (me and mi are the electron and ion masses, respectively). OSIRIS simulations also show that when crossing the shock, the upstream plasma is significantly heated The observed downstream wave spectrum is thus consistent with the hypothesis of a resonant interaction between electrons and ions being driven by lower-hybrid turbulence.

While the OSIRIS simulation indicates a significant heating of the plasma, because of finite computational resources, these are performed with an electron–ion mass ratio and plasma velocity different from that of the experiment. Thus, to apply the OSIRIS results to the measured data, the simulation conditions need to be properly re-scaled to those occurring in the experiment.

The average energy of electrons accelerated by lower-hybrid waves can be estimated9 by

$${E}_{e}={\alpha }^{2/5}{\left(\frac{{m}_{\rm{e}}}{{m}_{\rm{i}}}\right)}^{1/5}{m}_{\rm{i}}{u}^{2}$$

where α is an efficiency factor on the order of a few percent and u is the ion velocity (see Supplementary Information). Since OSIRIS simulations predict that lower-hybrid turbulence heats electrons to \({E}_{\rm{e}}^{{\rm{PIC}}} \sim 75\) keV, the rescaling to the laboratory conditions immediately follows from equation (1):


where we have assumed the same efficiency factor both in the laboratory and in OSIRIS simulations. The predicted average electron heating in the laboratory is ~ 45 eV, this electron energy can then be used in equation (1) to determine an efficiency factor of α ~ 0.1. Our OSIRIS simulation suggests that these accelerated electrons have a nearly Gaussian spectrum. The high-energy tail of this distribution is then responsible for the observed X-ray excess.

The collisional-radiative code PrismSPECT was used to calculate the X-ray emission from the predicted hot-electron population of lower-hybrid electrons (see Supplementary Information). When no hot population was present, no fluorine X-rays were obtained. As the efficiency factor α increases, the X-ray intensity of the observed fluorine line also increases (see Fig. 5). The PrismSPECT results show that an average hot-electron energy of at least 30 eV is sufficient to produce the X-rays observed within the laboratory.

Fig. 5: Atomic transition simulations.
Fig. 5

Results from PrismSPECT (purple line) indicate that as the hot-electron population is increased in both fraction and average energy according to the efficiency factor α from equation (1), the logged intensity of the fluorine He-α line also increases (the average electron energy for a given value of α is shown on the top horizontal axis for reference). When no hot-electron population is present, no fluorine He-α line is generated. There is minimal contribution from Bremsstrahlung. The average hot-electron energy (Ee ~ 45 eV) and efficiency factor (α ~ 0.1) for laboratory conditions is indicated with the black dashed line.

In the experiment, the counter-streaming fluorine ions have a collisional mean-free-path of ~ 5 mm (see Supplementary Information), to be compared with their gyroradius ~ 2 cm. This does not affect the growth of the lower-hybrid instability13.

Our results provide compelling evidence that lower-hybrid waves play an important role in energizing electrons, and thus provide a potential mechanism for overcoming the injection problem for perpendicular shocks. We infer the presence of this electron energization by the observation of excess X-ray emission from the plasma when a magnetized sphere is present. The magnetized sphere permits the generation of lower-hybrid waves through a shock-reflected ion instability, thus allowing these waves to energize the electrons by energy transfer from the ionic motion. While this electron energization process has been inferred in many astrophysical environments, it is not fully understood, and so makes our experiment an important platform for the validation of the particle acceleration models frequently invoked to explain the high-energy electrons observed at strong astrophysical shocks.


Lower-hybrid waves and modified two-stream instability

Lower-hybrid waves are electrostatic ion waves that propagate quasi-perpendicularly to an external magnetic field. Lower-hybrid waves have a frequency between the ion and electron gyro frequency and can be generated through a plasma instability, namely the modified two-stream instability (MTSI)13. The MTSI is similar to the two-stream instability in the sense that it is formed through counter-streaming flows; however, unlike the classic two-stream instability, the MTSI requires an external magnetic field oriented quasi-perpendicularly to a counter-streaming ion flow6.

This instability excites lower-hybrid waves, which have the following dispersion relation24:

$${\omega }^{2}={\omega }_{{\rm{LH}}}^{2}{\left(1+\frac{{\omega }_{\rm{pe}}^{2}}{{k}_{\perp }^{2}{c}^{2}}\right)}^{-1}\left(1+{x}^{2}\right)$$

where ωLH is the lower-hybrid frequency,

$${\omega }_{{\rm{LH}}}=\sqrt{\frac{{\omega }_{\rm{ci}}{\omega }_{\rm{ce}}}{1+{\left(\frac{{\omega }_{\rm{ce}}}{{\omega }_{\rm{pe}}}\right)}^{2}}}$$

and x is defined by

$${x}^{2}=\frac{{m}_{\rm{i}}}{{m}_{\rm{e}}}\frac{{k}_{\parallel }^{2}}{{k}_{\perp }^{2}}{\left(1+\frac{{\omega }_{\rm{pe}}^{2}}{{k}_{\perp }^{2}{c}^{2}}\right)}^{-1}$$

and ωpe is the electron plasma frequency, k|| and k are the components of the wavevector k parallel and perpendicular to the magnetic field, ωce and ωci are the electron and ion cyclotron frequencies, and mi and me are the ion and electron masses.

These lower-hybrid waves can accelerate electrons through Cerenkov resonance. Since the lower-hybrid waves travel mostly perpendicularly to the magnetic field, this wavevector component is much larger than that of the wavevector parallel to the magnetic field. As a consequence, the lower-hybrid waves have a high phase velocity along the field lines that resonate with fast moving electrons as well as a low phase velocity across the field lines that resonate with the slow moving ions. Consequently energy can be transferred via the lower-hybrid waves from the ions travelling perpendicular to the magnetic field to electrons travelling parallel to the field. In this manner, counter-streaming ions in an external magnetic field can accelerate electrons to large energies, and so produce high-energy X-rays.

Within the laboratory experiment described here, a counter-streaming ion flow is set up by reflecting ions off of the shock created at the sphere. The reflected ions and remaining incoming ions can then produce the MTSI, and so generate lower-hybrid waves. Lower-hybrid waves have been previously observed both astrophysically10,11,12,25 and in the laboratory, mostly within fusion devices26,27,28.

Lower-hybrid waves in space plasmas

Turning to astrophysical environments, in the passing of a comet through the solar wind, as described in ref. 9, lower-hybrid waves have been invoked to explain cometary X-ray emission. In this scenario, which is equivalent to what is described in the main paper by our experiment, the interaction of the incoming solar-wind ions with the ions reflected by the cometary bow shock excites waves within the LH frequency range. Here, the photo-ionized cometary ions are accelerated by the v × B electric field, where B is the magnetic field of the solar wind and v is the relative velocity between the cometary ions and the solar wind. These so-called pick-up cometary ions form a beam in the solar wind. Electrons are heated by LH waves, producing a suprathermal electron population. This hot-electron population is estimated to have an average energy ~ 100 eV and maximum energy ~ 5 keV. These suprathermal electrons are then capable of generating Bremsstrahlung and K-shell radiation from excited ions: mostly C, N and O29.

An alternative explanation of the observed X-ray emission is offered by considering charge exchange processes30. In this scenario, the heavier ions in the solar wind exchange charges with the neutral gases in the comet20, resulting in stronger line emission. This is also supported by laboratory experiments using a beam ion trap20.

Although both lower-hybrid turbulence and charge-exchange can explain the X-ray emission in comets, only the former can account for the observed X-ray excess in our experiment. The charge-exchange mechanism can be ruled out as the dominant mechanism in our experiment since it places no restriction on the presence of a magnetic field. The laboratory data show a large excess in X-ray production only in the presence of a magnetic field perpendicular to the flow.

Comparison between the laboratory, space and simulation

While the properties of plasmas in laboratory and space environments are often vastly different, through appropriate scaling of the relevant parameters involved, a comparison between the two environments can be made. In Supplementary Table S1 the relevant plasma parameters for this experiment, a comet interacting with the solar wind, and the OSIRIS simulations performed for this experiment are compared. Since the properties of greatest interest are those relating to the production of lower-hybrid waves via the MTSI, the fluorine ions only have been considered. The parameters shown in Supplementary Table S1 for the interaction of a comet with the solar wind were chosen with the following considerations in mind. The expanding gas cloud surrounding a comet is mostly comprised of water and some carbon dioxide, meaning that the majority of the cometary ions involved are photo-ionized oxygen ions. The temperature of the ions varies in the range ~ 0.02–0.2 eV, and so a value of 0.1 eV seems appropriate. The solar wind comprises of a slow mode with speed ~ 100 km s−1. The solar wind contains a magnetic field of ~ 10–200 μG and has ion temperatures of ~ 1–10 eV with electron densities of 1–10 cm−3. The parameters in the OSIRIS simulations are scaled to an electron density that matches the electron density in the experiment.

Supplementary Table S1 shows that while many of the parameters such as cyclotron frequencies and gyro radii are very different between the laboratory and astrophysical cases, scaled quantities, such as the ratio of gyro radii to skin depth, are conversely fairly similar. The product of the lower-hybrid frequency, ωLH, and the ion-beam collision time, τie is one way of comparing the growth of the instability. Clearly, in collisionless situations such as space and in OSIRIS simulations, the large timescale between collisions makes this quantity much greater than in the mildly-collisional laboratory case. On the other hand, a comparison between the period of the lower-hybrid wave oscillations and the time it takes for an ion to interact with a lower-hybrid wave (either V/rgi or τie, depending on which quantity is smaller) is similar for all three cases.

Data availability

All raw and derived data used to support the findings of this work are available from the authors on request.

Additional information

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We thank all the LULI technical staff at École Polytechnique for their support during the experiment. The research leading to these results has received funding from the European Research Council under the European Community’s Seventh Framework Programme (FP7/2007-2013)/ERC grant agreements no. 256973 and 247039, AWE plc, the Engineering and Physical Sciences Research Council (grant numbers EP/M022331/1, EP/N014472/1, EP/N013379/1 and EP/N002644/1) and the Science and Technology Facilities Council of the United Kingdom. F.C. and L.O.S. acknowledge support from the European Research Council (InPairs ERC-2015-AdG 695088), FCT Portugal (grant no. PD/BD/114307/2016) the Calouste Gulbenkian Foundation and PRACE for awarding access to resource MareNostrum, based in Spain at the Barcelona Supercomputing Center. The PIC simulations were performed at the IST cluster (Lisbon, Portugal), and MareNostrum (Spain). This work was supported in part at the University of Chicago by the US DOE NNSA ASC through the Argonne Institute for Computing in Science under FWP 57789 and the US DOE Office of Science through grant no. DE- SC0016566. The software used in this work was developed in part by the DOE NNSA ASC- and DOE Office of Science ASCR-supported Flash Center for Computational Science at the University of Chicago.

Author information


  1. Department of Physics, University of Oxford, Oxford, UK

    • A. Rigby
    • , A. R. Bell
    • , J. E. Cross
    • , P. M. Kozlowski
    • , M. Oliver
    • , S. Sarkar
    • , P. Tzeferacos
    •  & G. Gregori
  2. GoLP/Instituto de Plasmas e Fusão Nuclear, Instituto Superior Técnico, Universidade de Lisboa, Lisbon, Portugal

    • F. Cruz
    •  & L. O. Silva
  3. Laboratoire pour l’Utilisation de Lasers Intenses, UMR7605, CNRS CEA, Université Paris VI Ecole Polytechnique, Palaiseau Cedex, France

    • B. Albertazzi
    • , J. R. Marques
    •  & M. Koenig
  4. Rutherford Appleton Laboratory, Chilton, Didcot, UK

    • R. Bamford
    • , C. Spindloe
    • , R. Trines
    •  & R. Bingham
  5. Departments of Planetary Sciences and Astronomy, University of Arizona, Tucson, AZ, USA

    • F. Fraschetti
  6. AWE, Aldermaston, Reading, UK

    • P. Graham
  7. Institute of Laser Engineering, Osaka University, Suita, Japan

    • Y. Hara
    • , T. Morita
    •  & Y. Sakawa
  8. Department of Physics, National Central University, Taoyuan City, Taiwan

    • Y. Kuramitsu
  9. Graduate School of Engineering, Osaka University, Suita, Japan

    • Y. Kuramitsu
  10. Department of Astronomy and Astrophysics, University of Chicago, Chicago, IL, USA

    • D. Q. Lamb
    • , P. Tzeferacos
    •  & G. Gregori
  11. The Blackett Laboratory, Imperial College London, London, UK

    • S. Lebedev
  12. Department of Physics, ETH-Zürich, Zürich, Switzerland

    • F. Miniati
  13. School of Mathematics and Physics, Queens University Belfast, Belfast, UK

    • B. Reville
  14. Niels Bohr Institute, Copenhagen, Denmark

    • S. Sarkar
  15. Department of Physics, University of Strathclyde, Glasgow, UK

    • R. Bingham


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  25. Search for R. Bingham in:

  26. Search for M. Koenig in:

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G.G., B.R. A.R.B., F.F., S.L., F.M., S.S. and R.Bi. conceived this project, which was designed by G.G., S.L. and M.K. The LULI experiment was carried out by A.R., B.A., J.E.C., Y.H., P.M.K., Y.K., J.R.M., T.M., M.O., Y.S. and M.K. The paper was written by A.R., F.C., B.R. and G.G. The data were analysed by A.R. Numerical simulations were performed by F.C. and P.T. Further experimental and theoretical support was provided by R.Ba., P.G., D.Q.L., C.S., R.T. and L.O.S.

Corresponding author

Correspondence to A. Rigby.

Supplementary information

  1. Supplementary Information

    Supplementary figures 1,2, Supplementary Table 1, Supplementary notes and supplementary references

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