Slow coarsening in jammed athermal soft particle suspensions

Slow coarsening in jammed athermal soft particle suspensions

R. N. Chacko Department of Physics, Durham University, Science Laboratories, South Road, Durham DH1 3LE, UK    P. Sollich University of Göttingen, Institute for Theoretical Physics, 37077 Göttingen, Germany King’s College London, Department of Mathematics, London WC2R 2LS, UK    S. M. Fielding Department of Physics, Durham University, Science Laboratories, South Road, Durham DH1 3LE, UK
July 3, 2019
Abstract

We simulate a densely jammed, athermal assembly of repulsive soft particles immersed in a solvent. Starting from an initial condition corresponding to a quench from a high temperature, we find non-trivial slow dynamics driven by a gradual release of stored elastic energy, with the root mean squared particle speed decaying as a power law in time with a fractional exponent. This decay is accompanied by the presence within the assembly of spatially localised and temporally intermittent ‘hot-spots’ of non-affine deformation, connected by long-ranged swirls in the velocity field, reminiscent of the local plastic events and long-ranged elastic propagation that have been intensively studied in sheared amorphous materials. The pattern of hot-spots progressively coarsens, with the hot-spot size and separation slowly growing over time, and the associated velocity correlation length increasing as a sublinear power law. Each individual spot however exists only transiently, within an overall picture of strongly intermittent dynamics.

The physics of amorphous yield stress materials such as colloids, microgels, onion surfactants, star polymers, emulsions and foams has been the focus of intense research in recent years Bonn et al. (2017). Among such systems, an important sub-distinction is whether any given material is thermal or athermal. Indeed, hard sphere (or Lennard Jones) colloids that are small enough to experience Brownian motion undergo a thermal glass transition above a packing fraction . In contrast, soft particles (or droplets or bubbles) with radii m large enough for Brownian motion to be negligible undergo an athermal jamming transition above a packing fraction  Ikeda et al. (2012).

The rheological (deformation and flow) properties of these two classes of system have been intensively studied, in particular under an applied shear flow. For thermal glasses, the flow curve of shear stress versus shear rate exhibits a yield stress for packing fractions , where is the particle radius, Boltzmann’s constant, and the temperature. Athermal soft suspensions instead show a yield stress for , where is the particle modulus. At nonzero one then sees a crossover between these two limiting classes Ikeda et al. (2012). At the level of understanding the microscopic dynamics within the flowing material, the basic physical picture to have emerged is one of localised plastic “Eshelby” rearrangement events connected by long ranged elastic “Oseen” propagation Tanguy et al. (2006); Falk and Langer (1998); Chattoraj and Lemaitre (2013); Chikkadi et al. (2011); Picard et al. (2004); Schall et al. (2007); Desmond and Weeks (2015). At low temperatures and shear rates, these plastic events organise into system-spanning avalanches that flicker in and out of existence across the sample Salerno et al. (2012); Maloney and Lemaître (2006); Lemaître and Caroli (2007); Bailey et al. (2007); Dasgupta et al. (2012); Lin et al. (2014); Puosi et al. (2014); Liu et al. (2016).

The behaviour of thermal colloidal glasses has also been studied in detail even in the absence of any externally imposed flow Hunter and Weeks (2012). These materials display slow relaxation dynamics characterised by the power law decay of one-time quantities, and ageing in two-time quantities such as the self-intermediate scattering function or mean squared particle displacement. Thermally activated local plastic events analogous to those in flowing systems have also been identified Lemaître (2014).

In contrast, the physics of athermal soft suspensions in the absence of any externally imposed flow has been assumed trivial to date. Lacking as these materials do any thermal agitation, it has been generally assumed that they should jam up exponentially quickly, on a timescale set by the interparticle solvent viscosity divided by the particle modulus, with each particle rapidly attaining a local energy minimum relative to its neighbours. Indeed, a theoretical search for slow relaxation modes in athermal foams proved fruitless Buzza et al. (1995). Nonetheless, experimentally measured viscoelastic spectra in foams of typical bubble diameter m do reveal characteristically flat loss moduli down to the lowest accessible frequencies, indicating the presence of very slow relaxation modes Khan et al. (1988). (In foams one cannot however rule out a slow increase in bubble size over time: a relaxation mechanism that is absent for the soft particles simulated here.)

The contribution of this Letter is to show, for the first time theoretically, that athermal suspensions of soft particles do show non-trivial dynamics, even in the absence of an externally imposed flow (or changes in particle size). Following sample preparation at some initial time in a state with packing fraction , we demonstrate a scenario of slow dynamics driven by a progressive decline of the stored mean particle elastic energy towards a final value . The associated rate of change decays as a power law with a fractional exponent , as does the root mean squared particle speed, . Such a scenario suggests that the dynamics within the assembly become correlated on progressively larger lengthscales as time proceeds. Indeed, we identify the presence of temporally intermittent and spatially localised ‘hot-spots’ of non-affine deformation, connected by long-ranged swirling velocity vortices, in a scenario reminisent of the Eshelby-Oseen dynamics of sheared amorphous materials Tanguy et al. (2006); Falk and Langer (1998); Chattoraj and Lemaitre (2013); Chikkadi et al. (2011); Picard et al. (2004); Schall et al. (2007); Desmond and Weeks (2015). The pattern of these hot-spots slowly coarsens over time, with the hot-spots gradually becoming larger and further apart, although each individual spot itself exists only transiently. The associated velocity correlation length grows as a sublinear power law, .

We simulate an athermal assembly of repulsive soft particles immersed in a solvent at high packing fraction, assuming a pairwise harmonic interparticle repulsive potential, , where is the Heaviside function. We take a bidisperse mixture of particles with radii and in equal number, with for any particle pair . Neglecting hydrodynamic interactions, we assume that the potential forces are balanced simply by drag against the solvent, with the position of the th particle obeying:

(1)

where is the drag coefficient. Such a simulation is intended to describe, for example, a dense emulsion, foam or microgel comprising droplets, bubbles or particles of typical radius m. Hereafter, we shall refer to bubbles and droplets also simply as particles.

Figure 1: Decay of the root mean squared particle speed in , for (curves upwards) and , for (curves upwards). Distributions of log particle speed for and , both for times and (curves leftward). Insets: Horizontally-shifted distributions to highlight the widening of the distributions with increasing time.

It should be noted that the form of drag in Eqn. (1), although used widely in the literature, violates Galilean invariance. However, we have checked that replacing it by the properly invariant (although still approximate) form used in dissipative particle dynamics Groot and Warren (1997) does not change the physical scenario that we shall report.

We integrate Eqn. (1) using an explicit Euler algorithm, with an adaptive timestep scaled by the inverse maximum particle speed, . All results are converged to the limit . We choose units of length in which the smaller particle radius , of time in which the drag coefficient , and of mass in which the particle modulus . The physical parameters that remain to be explored are then the packing fraction of the assembly, , and the spatial dimensionality, . We mostly present results below for but data not shown here demonstrate that the same physical scenario also holds for .

Two different initial conditions are considered. In the first, the particles are placed in the simulation box at time with uniformly distributed positions. Physically, this corresponds to a sudden quench to temperature from a previously infinite temperature. In the second, the assembly is initially equilibrated at a reduced volume fraction, , and nonzero temperature , by augmenting Eqn. (1) with a thermal noise term, before suddenly expanding the particles in situ at time to achieve the desired , and setting . This is intended to model the rapid swelling of core-shell particles to reach a jammed state. Beyond an initial transient up to a typical time, we find the same dynamical scenario including non-trivial power-law decays for both of these initial conditions. Accordingly, results will be presented only for the fully random initial condition.

Figure 2: Colour maps in rows downwards for times and of (left) particle speeds, (centre) non-affine deformation rate and (right) temporal rate of change of particle energy , normalised as . The colour scales for and are centred around the median of their logarithms.

We start by showing in Fig. 1 the decay of the root mean squared particle speed for a range of packing fractions from just below to far above . We do so for both (Fig. 1a), where and for (Fig. 1b), where . After an initial transient persisting to a time , the decay enters a power law regime. For packing fractions below jamming, , this power law is eventually cut off by a final exponential decay. Above jamming, , the power law persists to a time that increases without bound as the system size increases. (For any finite , it finally ends in noise. We show in Fig. 1 only -independent results.) We find an exponent in and in . In both cases the typical speeds therefore decay significantly more slowly than one would expect for trivial non-glassy decay towards a crystalline lattice, where a simple analytical calculation yields . The associated log-speed distribution gradually shifts to lower speeds overall, but with a tail for higher than average speeds that also broadens slightly, Fig. 1c–d.

The observation of a steadily slowing power law decay suggests that spatial correlations develop within the assembly on progressively larger lengthscales as time proceeds. To investigate this, we show in Fig. 2 snapshot colour maps of the particle speed , the temporal rate of change of particle energy (where is the potential energy contribution of particle ), and the non-affine part of the local deformation rate, which as an instantaneous version of Falk and Langer (1998) we define at each particle as

(2)

where the sum runs over neighbours within a maximum distance of . At any fixed time, localised hot-spots of high particle speed, rapidly changing particle energy, and high non-affine deformation rate are evident. With increasing time in rows downwards, the patterns coarsen, with the hot-spots becoming progressively larger and further apart. Each spot itself exists only transiently, however, with a dynamics that is highly intermittent in nature. We shall return to expand on this point below.

Figure 3: Zoom-in on a region for a two-dimensional system of particles at packing fraction . (a) Displacement field over the time interval to , scaled by a factor to improve visibility. (b–d) Evidence of propagation in the normalised local rate of energy change at times , and respectively, with colour scale linearly interpolating between (blue) and (red).

This scenario of spatially localised hot-spots is strongly reminiscent of the local plastic events (sometimes called shear transformation zones) that are widely discussed in the context of sheared amorphous materials Tanguy et al. (2006); Falk and Langer (1998); Chattoraj and Lemaitre (2013); Chikkadi et al. (2011); Picard et al. (2004); Schall et al. (2007); Desmond and Weeks (2015), and that also arise via thermal activation in unsheared colloids Lemaître (2014). Each such zone has been shown to create around itself a long-ranged elastic perturbation according to the Oseen propagator of linear elasticity, giving rise to long-ranged vortex-like structures in the velocity field. Strikingly similar behaviour is seen in our simulations: a typical map of displacement (integrated over a short time interval) is displayed in Fig. 3 and clearly resembles that of Fig. 3 of Ref. Maloney and Lemaître (2006) for a sheared amorphous material, with the overall imposed shear subtracted out.

Figure 4: Data for a two-dimensional system at at times and (from dark to light). (a) Normalized velocity correlation function. Inset: Characteristic lengthscale at which the velocity correlator falls below against time. Dashed line is a fit to a power law. (b) Exponent against , where is the mean-squared displacement of particles between times and . Top inset: against . Bottom inset: against , collapsing the ballistic parts of the curves.

To investigate further the structure of these swirling vortices, we show in Fig. 4a the spatial velocity correlation function, for values of time increasing in curves rightwards. Its characteristic decay length increases over time according to a power law where we estimate the exponent as in , Fig. 4a (inset).

So far, we have shown that the pattern of hot-spots slowly coarsens over time, with increasing hot-spot size and separation, and a growing velocity correlation length . Alongside this basic picture, we now further demonstrate the dynamics to be strongly intermittent, with each individual hot-spot itself existing only transiently. To do so, we show in Fig. 5a,b the temporal signals of non-affine deformation rate, and the rate of change of particle energies, for four randomly chosen particles. Each particle clearly experiences intervals of relative quiescence punctuated by bursts of high local activity. The correlation between local non-affinity and rate of change of particle energy that is visually apparent in the time signals of Fig. 5a,b is demonstrated quantitatively in the contour plot of Fig. 5c.

To summarise, we have demonstrated a scenario of non-trivial slow dynamics in a dense athermal suspension of purely repulsive soft particles, with the mean squared particle speed decaying over time as a sublinear power law. This contrasts with the naive intuition that any such system should quickly jam up as each particle rapidly attains a local energy minimum relative to its neighbours, and indicates that collective effects become increasingly dominant over time, on progressively larger lengthscales. Consistent with this expectation, we have demonstrated the existence within the assembly of hot-spots of locally non-affine deformation, linked by long ranged swirls in the velocity field, in a scenario reminiscent of the local plastic events and elastic stress propagation that has been intensively studied in sheared amorphous materials. The pattern of hot spots slowly coarsens over time, with the associated velocity correlation length increasing as a sublinear power law.

There is clearly significant scope for further investigation of the non-trivial aging dynamics we have identified in athermal systems. The structure and growth of the hot-spots would be interesting to study, for example. Here, as the system descends in its potential energy landscape, less and less energy is available to ‘activate’ plastic rearrangements over local energy barriers. One would then conjecture that these plastic rearrangements, which take place within the hot-spots, become increasingly collective in order to reduce the height of the corresponding energy barriers. The spectrum and properties of instantaneous normal modes during the aging process will also be interesting to study, in particular in relation to existing results for statically jammed or driven athermal systems O’Hern et al. (2001); Liu and Nagel (2010) Finally, the consequences of athermal aging for the rheology (mechanical behaviour) will be fascinating to explore. This will provide non-trivial benchmarks on which to test and refine existing mesoscopic modelling approaches Hébraud and Lequeux (1998); Sollich et al. (2017, 1997); Falk and Langer (2011) in the relevant athermal regime. It will also help us to understand the qualitative differences and commonalities with aging in thermal, largely entropy-driven glasses such as colloidal hard spheres, where mode-coupling theory has been shown to be a useful modelling paradigm van Megen and Pusey (1991); Brader et al. (2009); Kob (1997).

Figure 5: (a) Time signal of the non-affine deformation rate, defined in Eqn. (2) for four particles, labelled by colour. These were chosen out of one hundred randomly selected particles such that their dynamics is of a similar scale. (b) Corresponding signal of the rate of change of particle energy for the same three particles. (c) Correlation of the non-affine deformation rate with the absolute rate of change of particle energy at time . Contours show level sets for the number of particles, , within bins of width and height in -space. Data shown for packing fraction in two dimensions, .

Acknowledgements — The authors thank Mike Cates and Ricard Matas Navarro for useful discussions. The research leading to these results has received funding from SOFI CDT, Durham University, from the EPSRC (grant ref. EP/L015536/1) and from the European Research Council under the European Union’s Seventh Framework Programme (FP7/20072013) / ERC grant agreement number 279365.

References

  • Bonn et al. (2017) D. Bonn, M. M. Denn, L. Berthier, T. Divoux,  and S. Manneville, Reviews of Modern Physics 89, 035005 (2017).
  • Ikeda et al. (2012) A. Ikeda, L. Berthier,  and P. Sollich, Physical Review Letters 109, 018301 (2012).
  • Tanguy et al. (2006) A. Tanguy, F. Leonforte,  and J.-L. Barrat, European Physical Journal E 20, 355 (2006).
  • Falk and Langer (1998) M. L. Falk and J. S. Langer, Physical Review E 57, 7192 (1998).
  • Chattoraj and Lemaitre (2013) J. Chattoraj and A. Lemaitre, Physical Review Letters 111, 066001 (2013).
  • Chikkadi et al. (2011) V. Chikkadi, G. Wegdam, D. Bonn, B. Nienhuis,  and P. Schall, Physical Review Letters 107, 198303 (2011).
  • Picard et al. (2004) G. Picard, A. Ajdari, F. Lequeux,  and L. Bocquet, European Physical Journal E 15, 371 (2004).
  • Schall et al. (2007) P. Schall, D. A. Weitz,  and F. Spaepen, Science 318, 1895 (2007).
  • Desmond and Weeks (2015) K. W. Desmond and E. R. Weeks, Physical Review Letters 115, 098302 (2015).
  • Salerno et al. (2012) K. M. Salerno, C. E. Maloney,  and M. O. Robbins, Physical Review Letters 109, 105703 (2012).
  • Maloney and Lemaître (2006) C. E. Maloney and A. Lemaître, Physical Review E 74, 016118 (2006).
  • Lemaître and Caroli (2007) A. Lemaître and C. Caroli, Physical Review E 76, 036104 (2007).
  • Bailey et al. (2007) N. P. Bailey, J. Schiøtz, A. Lemaître,  and K. W. Jacobsen, Physical Review Letters 98, 095501 (2007).
  • Dasgupta et al. (2012) R. Dasgupta, H. G. E. Hentschel,  and I. Procaccia, Physical Review Letters 109, 255502 (2012).
  • Lin et al. (2014) J. Lin, E. Lerner, A. Rosso,  and M. Wyart, Proceedings of the National Academy of Sciences 111, 14382 (2014).
  • Puosi et al. (2014) F. Puosi, J. Rottler,  and J.-L. Barrat, Physical Review E 89, 042302 (2014).
  • Liu et al. (2016) C. Liu, E. E. Ferrero, F. Puosi, J.-L. Barrat,  and K. Martens, Physical Review Letters 116, 065501 (2016).
  • Hunter and Weeks (2012) G. L. Hunter and E. R. Weeks, Reports on Progress in Physics 75, 066501 (2012).
  • Lemaître (2014) A. Lemaître, Physical Review Letters 113, 245702 (2014).
  • Buzza et al. (1995) D. Buzza, C.-Y. Lu,  and M. Cates, Journal de Physique II 5, 37 (1995).
  • Khan et al. (1988) S. A. Khan, C. A. Schnepper,  and R. C. Armstrong, Journal of Rheology 32, 69 (1988).
  • Groot and Warren (1997) R. D. Groot and P. B. Warren, Journal of Chemical Physics 107, 4423 (1997).
  • O’Hern et al. (2001) C. S. O’Hern, S. A. Langer, A. J. Liu,  and S. R. Nagel, Phys Rev Lett 86, 111 (2001).
  • Liu and Nagel (2010) A. J. Liu and S. R. Nagel, Annu. Rev. Condens. Matter Phys. 1, 347 (2010).
  • Hébraud and Lequeux (1998) P. Hébraud and F. Lequeux, Phys Rev Lett 81, 2934 (1998).
  • Sollich et al. (2017) P. Sollich, J. Olivier,  and D. Bresch, J. Phys. Math. Theor. 50, 165002 (2017).
  • Sollich et al. (1997) P. Sollich, F. Lequeux, P. Hébraud,  and M. E. Cates, Phys Rev Lett 78, 2020 (1997).
  • Falk and Langer (2011) M. L. Falk and J. S. Langer, Annu. Rev. Condens. Matter Phys. 2, 353 (2011).
  • van Megen and Pusey (1991) W. van Megen and P. N. Pusey, Phys Rev A 43, 5429 (1991).
  • Brader et al. (2009) J. M. Brader, T. Voigtmann, M. Fuchs, R. G. Larson,  and M. E. Cates, PNAS 106, 15186 (2009).
  • Kob (1997) W. Kob, ACS Symp Ser 676, 28 (1997).
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