1. Introduction
Understanding and theoretically describing the static/flowing transition in dense granular flows is a central issue in research on granular materials, with strong implications for industry and geophysics, in particular in the study of natural gravity-driven flows. Such flows (e.g., landslides or debris avalanches) play a key role in erosion processes on the Earth’s surface and represent major natural hazards. In recent years, significant progress in the mathematical, physical, and numerical modeling of gravity-driven flows has made it possible to develop and use numerical models for the investigation of geomorphological processes and assess risks related to such natural hazards. However, severe limitations prevent us from fully understanding the processes acting in natural flows and predicting landslide dynamics and deposition, see e.g., [
1]. In particular, a major challenge is to accurately describe complex natural phenomena such as the static/flowing transition.
Geophysical, geotechnical, and physical studies have shown that the static/flowing transition related to the existence of no-flow and flow zones within the mass plays a crucial role in most granular flows and provides a key to understanding their dynamics in a natural context, see [
1] for a review. This transition occurs in erosion-deposition processes when a layer of particles flows over a static layer or near the destabilization and stopping phases. Note that natural flows often travel over deposits of past events, which may or may not be made of the same grains, and entrain material from the initially static bed. Even though erosion processes are very difficult to measure in the field, e.g., [
2,
3,
4], entrainment of underlying material is known to significantly change the flow dynamics and deposition, e.g., [
5,
6,
7,
8,
9,
10].
Experimental studies have provided some information on the static/flowing dynamics in granular flows, showing for example that the presence of a very thin layer of erodible material lying on an inclined bed may increase the maximum runout distance of a granular avalanche flowing down the slope by up to
and change the flow regimes [
9,
11,
12]. In these experiments that mimic natural flows over initially static beds (
Figure 1), quasi-uniform flows develop when the slope angle
is a few degrees lower than the typical friction angle
of the involved material [
12].
Figure 2 and
Figure 3 show new data extracted from the experiments performed by [
12] on the change with time of the static/flowing interface position
b and the velocity profiles
within the granular mass, where
Z is the direction normal to the bed. At a given position
X along the plane, the flow is shown to excavate the initially static layer immediately when the front reaches this position. The static/flowing interface rapidly penetrates into the static layer, reaching a lowest position (that depends on the slope angle) for significantly high slopes and then rises almost linearly or exponentially toward the free surface until the whole mass of material stops (
Figure 2). A theoretical description of these observations is still lacking. In particular, questions remain as to what controls the change with time of the static/flowing interface position and the velocity profiles and how these characteristics are related to the rheology of the granular material and the initial and boundary conditions.
In order to alleviate the high computational costs required to describe the real topography and the rheology, which both play a key role in natural flow dynamics, thin-layer (i.e., the thickness of the flow is assumed to be small compared to its down-slope extension) depth-averaged models are generally used to simulate landslides [
14]. Such models have been rigorously derived for arbitrary topography, but the static/flowing transition has generally been neglected, e.g., [
15,
16,
17,
18]. Several attempts have been made to describe this transition in thin-layer (i.e., shallow) models, in particular by deriving an equation for the static/flowing interface position or by establishing erosion/deposition rates, e.g., [
19,
20]. However, these approaches are generally based on debatable phenomenological laws and/or are too schematic to be extended to natural flows [
21]. The simplifications used in some previous models lead to an inconsistent energy Equation [
22]. Indeed, some of these models prescribe a given velocity profile to deduce the entrainment rate (see e.g., [
23] or references in [
22]). However, in transient flows, the velocity profile changes with time as shown for example in the multilayer shallow model of [
24]. A better understanding of the non-averaged case is necessary before defining more physically relevant depth-averaged models including the static/flowing transition. This is why we focus here on non-averaged thin-layer models.
Recent work has shown that viscoplastic flow laws with yield stress describe well granular flows and deposits in different regimes, from steady uniform flows [
25,
26,
27,
28] to transient granular collapse over rigid or erodible horizontal beds [
29,
30,
31] and inclined beds [
24,
32,
33] or accelerating/decelerating channel flows [
34]. Very good agreement with experiments is obtained even though these laws, and in particular the so-called
rheology, where
I is the inertial number [
28], have been shown to be ill-posed in the quasi-static regime, i.e., for small
I (and also for large
I) [
35]. These promising results may be related to the use of a coarse mesh, whereby simulations avoid the ill-posedness by damping the fast-growing high wavenumbers [
33]. In any case, the quasi-static regime near the static/flowing interface is known to be very complex, involving strong and weak force chains and local rearrangement of particles, e.g., [
36,
37] and has been widely studied, in particular using discrete element methods, e.g., [
1,
38,
39]. This regime is not accurately described by the proposed viscoplastic laws involving a simple yield stress. Questions however remain as to whether such ‘simple’ viscoplastic laws are able to describe quantitatively the change with time of the static/flowing interface position and the velocity profiles observed experimentally for flows over an initially static bed and how the viscosity affects these processes.
Based on such a viscoplastic model with yield stress, an analytic expansion in the non-averaged thin-layer regime is provided in [
40], giving a theoretical basis for equations describing the static/flowing interface dynamics in a dry granular material. A key point in this approach that fundamentally differs from previous thin-layer models (see [
21] for a review) is that even if the flow is assumed to be thin, the normal coordinate
Z is still present (there is no depth-averaging). The static/flowing interface is free in this approach, in the sense that it has no explicit equation defining its evolution. Its time variation is instead implicitly determined by an extra boundary condition on the velocity at this interface. The model from [
40] being still too complicated, however a formal decoupling of the coordinates
X in the down-slope direction and
Z normal to the topography is proposed in [
41], leading to a model with only the coordinate
Z, but including a source term
S that represents the opposite of the net force acting on the flow, including gravity, pressure gradient, and internal friction. We propose here to evaluate the dynamics produced by the free interface model of [
41], for the most simple case involving a constant source
S. This corresponds to assuming no dependency on the down-slope coordinate
X in the model of [
40]. It is also equivalent to considering simple shear solutions to the original viscoplastic model, which shows that in this case the model is valid without a smallness assumption. Although the down-slope coordinate
X plays a key role in real flows, taking into account the fluctuations of the free surface, topography, and inflow information, we must first understand the dynamics when
X is not involved. We show that the analysis of this simple shear system provides new insight into the change of the static/flowing interface position and the velocity profiles with time.
Because the boundary conditions and interface evolution are formulated in an uncommon way, specific methods must be used to deal numerically with the free interface model. We introduce two numerical methods that give similar grid-independent results, thereby showing that our model is well-posed for the case considered here involving only Z dependency.
The paper is organized as follows. The model of [
40,
41] for the case of a constant source (corresponding to simple shear flows of the viscoplastic model) is recalled in
Section 2. Then, in
Section 3, we derive an analytical solution for the inviscid model with a constant source term, which partly reproduces the experimental observations and shows explicitly how the static/flowing interface position and the velocity profiles are related to the flow characteristics and to the initial and boundary conditions. In
Section 4, we introduce two new numerical methods for the simulation of the viscous model, with a constant viscosity or the variable viscosity associated with the
rheology. The numerical results show that, as opposed to the inviscid model, viscosity makes it possible to reproduce the initial penetration of the static/flowing interface within the static bed and the exponential shape of the velocity profiles near this interface. Finally, in
Section 5, these results are discussed based on comparison with former experimental and numerical studies on granular flows, showing the key features and the limits of the non-averaged thin-layer model for providing a better understanding and modeling of laboratory and natural flows.
4. Numerical Solution to the Viscous Free Interface Model
In this section, we consider a numerical solution to the free interface model (3)–(6) with viscosity and constant and uniform source term S given by (14). We first present two robust numerical methods to obtain the numerical solution. Then, we describe the main features of the transient regime by a scale analysis. Finally, we compare our numerical results with experiments, first with constant viscosity and then with variable viscosity deduced from the viscoplastic rheology.
Given the unusual form of our model with a free moving interface, some comments are in order. From the mathematical standpoint, it is not obvious that the boundary formulation (4) gives a well-posed problem. Actually, it is known [
35] that the
rheology can lead to an ill-posed problem. We claim that for the simple shear configuration considered here, the model is well-posed (although this would not be the case if
X dependency were involved, see [
40]). To support this claim, we observe that we consider two different numerical methods which both deliver stable, grid-independent solutions. Moreover, the second numerical method is related to an optimal problem under a very classical form (see (26) below), for which well-posedness is well-known. From a numerical standpoint, we point out that both numerical methods are computationally effective. Let us mention in passing that none of these methods uses the differential Equation (8) which would require an intricate treatment of the third-order derivative, but use instead the boundary conditions (4).
4.1. Discretization by Moving the Interface
The first numerical method involves rewriting (3), (4), (5) for a normalized coordinate
. We perform the change of coordinates
that leads to the differential relations
and
. Here,
and
denote the differentiation with respect to time at constant
Z and
Y, respectively. The change of coordinates (19), and hence the discretization method presented in this subsection, is appropriate as long as there is a flowing layer so that
. Another discretization method dealing with the stopping phase when
reaches the total height
h is presented in
Section 4.2. The discretization method considered in this subsection has the advantage of tracking explicitly the position of the static/flowing interface, whereas the method of
Section 4.2 requires post-processing to evaluate the interface position.
Using the change of coordinates (19), Equation (3) becomes
and the boundary conditions (4) become
We split the space domain
into
cells of length
with
and denote the center of the cells by
, for all
. For
, the discrete times
are related by
, where
is the time step (chosen according to the CFL condition (25) below) and
. We write a finite difference scheme for the discrete unknowns
and
, for all
and all
, using the initial conditions
(and
) to initialize the scheme. For all
, given
and
, the equations to compute
and
are
for all
, with
together with the boundary conditions
In Equation (22), the values
are assumed to be known, and they are computed as interface values from a given variable viscosity
. Equations (24a) and (24c) are used to provide the ghost values
and
needed in Equation (22) for
and
, respectively, whereas Equation (24b) is used to determine
as described below. We observe that in Equation (22), the diffusive term is treated implicitly in time, and the first-order derivative of
U is treated explicitly using upwinding. As a result, we impose the CFL condition
This CFL condition is evaluated approximately using the value from the previous time step, since is unknown at the beginning of the time step; for , the value 0 is used (hence, no CFL condition is initially enforced, but the time step is taken small enough). Typical values are s for the initial time step and .
The solution to Equations (22)–(24) is obtained as follows. We can solve the system (22) together with the boundary conditions (24a) and (24c) for any value of
since it is a linear system in
with right-hand side containing
, the source term and the advection term (remember that the advective derivative is treated explicitly). This leads to a tridiagonal linear system with a matrix that results only from the time derivative and the diffusive terms. This matrix, which is diagonally dominant, has an inverse with nonnegative entries. Thus, the solution
can be expressed linearly with nonnegative coefficients in terms of the coefficients
which appear on the right-hand side and which depend on the still unknown interface position
. According to (23) and since
is nondecreasing with respect to
j (it should remain nondecreasing because we assume
),
is thus, for all
, a nondecreasing continuous and piecewise linear function of
, with two different formulae corresponding to whether
is greater or smaller than
. In particular, the remaining boundary condition (24b), which is equivalent to
owing to (24a), determines a unique solution
, see
Figure 8. The value of
can be computed explicitly by solving the linear system twice with two different right-hand sides and using linear interpolation. The first solve uses the right-hand side evaluated with the temporary value
for
, yielding a temporary value for
. If the obtained value is negative (left panel of
Figure 8), the second solve is performed using the value
h for
, otherwise the value 0 is used (right panel of
Figure 8). Once
is known, we determine the entire profile
for all
by linear interpolation.
4.2. Discretization by an Optimality Condition
The second numerical method for solving conditions (3), (4) and (5) with positive viscosity
uses a formulation as an optimal problem set on the whole interval
, valid under the assumption
,
where we consider a no-slip boundary condition at the bottom. Note that this condition becomes relevant whenever the static/flowing interface reaches the bottom, a situation encountered in our simulations as shown in Figure 10c. In (26), the static/flowing interface position
no longer appears explicitly, but has to be deduced from the velocity profile as
We split the space domain
into
cells of length
with
, and denote the center of the cells by
, for all
. The discrete times
, for all
, are related by
, where
is the time step (chosen according to the CFL condition (30) below) and
. We discretize the problem (26) using a finite difference scheme by writing for the discrete unknowns
for all
. The boundary conditions, which are discretized as
at the free surface (
) and as
at the bottom (
), are used to provide the ghost values involved in the discretization of the diffusive term. The problem (28) is solved in two steps as
Owing to the explicit discretization of the diffusive term, we use the CFL condition
We could also consider an implicit discretization to avoid any CFL condition, but each time step would be more computationally demanding. Finally, the thickness of the static layer can be evaluated as
However, to prevent
from being influenced by small values of
U and for better accuracy, we prefer to use
where
is an appropriate constant of the order of
, in relation to Equations (4a), (4b) and (7).
In our computations, we use 200 space cells. With the value m, this leads to m. Since ms ms ms, this gives a velocity threshold of ms. This value is much smaller than the accuracy of experimental velocity measurements which is around 1 cm/s.
4.3. Scales in the Transient Regime
We assume that the source term
S is constant, and that the viscosity
is also constant. Then, the solution to the viscous model (3)–(5) depends on the constant
S, the total thickness
h, the viscosity
, the initial thickness of the static layer
, and the initial velocity profile
. We introduce dimensionless quantities, denoted by carets (hats),
where
is a time scale,
l a space scale, and
with
being the order of magnitude of the initial shear rate. In order to write Equation (3) in dimensionless form, we take
The dimensionless equation is then
with boundary conditions
at
and
at
. If we take a linear initial velocity profile, this dimensionless solution
depends only on
and
. Actually, since the problem is invariant by translation in
Z, the solution depends only on
.
Numerical investigations for a constant source
S using the scheme described in
Section 4.1 show the behavior illustrated in
Figure 9. The static/flowing interface position
first decreases until a time
and reaches a minimal value
(starting phase). Then
increases and (if
h is sufficiently large) reaches an asymptotic regime with upward velocity
(stopping phase), before fully stopping when it reaches
h.
According to the above scaling analysis, if the velocity profile is initially linear with shear
, and if
then the dimensionless problem has no parameter left and the velocity
is therefore a fixed profile (in terms of
), as well as
. We conclude with (33) that the quantities
,
,
are proportional to
,
l,
, respectively. We obtain the following proportionality factors from the numerical simulation
Note the dependency on the ratio , which is due to the homogeneity of the problem (3) and (4) with respect to (a new solution can be obtained by multiplying by a positive constant, with b unmodified).
4.4. Results and Comparison with Experiments for Constant Viscosity
We consider a constant and uniform source term of the form (14). The case of a linear initial velocity profile is simulated using different values of the viscosity
(taken constant) and slope angles
. The results obtained with the two methods of
Section 4.1 and
Section 4.2 are always identical, thus we shall not specify which one is used. As discussed in
Section 4.3, the static/flowing interface always penetrates the initially static layer, in contrast to what has been observed for the inviscid model, within a length
proportional to
, according to (36). In other words, the flow excavates the static bed. However, for
m
s
, the penetrating length is too small to be observed. For
m
s
(
Figure 10a),
m for
(with
s) and
m for
(with
s). Thus, the static/flowing interface penetrates only slightly within the initially static layer. As the viscosity increases (
Figure 10b), the static/flowing interface penetrates deeper into the initially static layer and even reaches the bottom for
m
s
at
(
Figure 10c). The results that best reproduce the experimental observation for the penetration of
within the initially static layer are obtained with
m
s
. In good agreement with the experiments, the simulations with viscosity predict that the depth and duration
of penetration of the static/flowing interface within the initially static layer increase with the slope angle. Furthermore, the values of
and
are in reasonable agreement with those observed experimentally (Figure 10b and Figure 17 of [
12]).
Qualitatively similar results are obtained using different initial velocity profiles (Figure 12). However, the shape of
is affected by the choice of the initial velocity profile. For example, for an exponential initial velocity profile with
and
m
s
, the static/flowing interface position
stagnates at an almost constant position for the first 0.5s, contrary to the case of a linear initial velocity profile (
Figure 10b and Figure 12b).
The convex shape of
during the migration of the static/flowing interface up to the free surface obtained with the viscous model is very different from that observed and from that obtained with the inviscid model, which predicted a linear shape related to the linear initial velocity profile. With the viscous model, the time evolution of
and the velocity profile
are not so clearly related to the shape of the initial velocity profile, as shown for example in Figure 12 for
. The velocity profiles for the viscous model are also very different from those for the inviscid model. Whatever the shape of the initial velocity profile, the velocity profiles later exhibit an exponential-like tail near the static/flowing interface, similar to that observed experimentally. They also exhibit a convex shape near the free surface which can be observed, although not as marked, in some but not all experimental velocity profiles (e.g.,
Figure 3c). While the maximum velocity decreases too fast at
s and
compared to the experiments and to the inviscid model, the velocity is much closer to the experiments at
s than with the inviscid model (
Figure 11b). For
and
, the decrease in velocity at time
s is overestimated in the viscous model.
Finally, we briefly look at the stopping time
of the whole granular layer. The stopping time for the inviscid model and for the experiments is given in
Table 1, for different slope angles. The stopping time is smaller for viscous than for inviscid flow, whatever the shape of the initial velocity profile. Given that the stopping time for the inviscid model is expressed as
, we can evaluate numerically the difference
, where
denotes the stopping time for the viscous model. Our numerical simulations show that this difference depends to a moderate extent on the viscosity (
Figure 13 where the slope of the curves suggests a behavior of this difference close to
for the present parameters). In any case, the presence of viscosity diminishes the stopping time. Consequently, according to
Table 1, the stopping time is significantly smaller in the viscous model than in the experiments. This can also be observed in
Figure 10 and
Figure 12 (right).
4.5. Variable Viscosity
The viscoplastic description of granular materials involves fundamentally a Drucker-Prager yield stress proportional to the pressure, the coefficient being the static friction parameter
. A full rheological law including this yield stress (i.e., defined for all values of the strain rate and not only close to zero) has been proposed in [
28], the so called
rheology. As described in [
32], this rheology can be interpreted as a decomposition (i.e., (2)) of the deviatoric stress tensor in a rate-independent pure plastic part proportional to
and a viscous part with pressure- and rate-dependent dynamic viscosity
given by
where
is the dynamic pressure,
D is the strain rate tensor,
, and
I is the inertial number defined by
with
d the grain diameter as before and
the grain density. The kinematic pressure
p is related to
by
, with
the density of the granular material,
being the volume fraction. If we consider a slope aligned velocity field depending only on the normal coordinate
Z (simple shear flow), the arguments of
Section 2.3 show that the solution to the viscoplastic model (1) and (2) is described by the system (3)–(5) with the constant and uniform source term
S given by (14) and
. Such a flow has hydrostatic pressure
and shear rate
. Thus with (37), the kinematic viscosity becomes
with
Then the term appearing in (3) is
and the part of this term proportional to
indeed balances in (3) the corresponding part in
S from (14). The nonlinearity is given according to [
28] as
with
the friction at large strain rate and
is a constant that depends on the material used and other device specificities, see ([
27], Appendix A). Here we take the value
proposed by [
27]. Note that the boundary condition (4c) is automatically satisfied and can therefore be skipped.
For the discretization, we use the method of
Section 4.2 with the discrete unknowns
,
for
,
. The Equations (3) and (41) with (42) and (40) are discretized with finite differences under the conservative form
for all
, with
for
, with
, and once
has been computed, we set
Since , there is no need to define , in accordance with the loss of the free surface boundary condition (4c). On the left boundary (bottom), we use as before the no-slip condition, . We use the CFL condition , with defined as the maximum value of computed with (39). The interface position is computed according to (32).
As previously, we take
,
m,
m, and
m. As in [
12], we take
. We choose
, which leads to
m
s
, corresponding to the order of magnitude of
taken in
Section 4.4. We consider the case of a linear initial velocity profile, with slope angles
. The numerical results for the static/flowing interface position
and velocity profiles
are plotted in
Figure 14 and
Figure 15. In comparison with numerical results of
Figure 10b and
Figure 11a,b obtained with the constant viscosity model, the shapes are similar, in particular for the initial erosion of the static bed. The behavior of the interface position
reaching the free surface close to the stopping time is here closer to the prediction of the inviscid model (see
Figure 5a). However, this behavior does not recover (since
vanishes at the free surface) the expected behavior, which is roughly linear, of the experimental results of
Figure 2. The comparison with the experimental results is better with the
rheology than with a constant viscosity. For clarity, the static/flowing interfaces and the velocity profiles corresponding to the different cases are plotted in
Figure 16 for
.
It is important to explain the behavior of the solution close to the free surface. As said above, there is no need to impose any boundary condition at the free surface, because the pressure vanishes there. Nevertheless, the behavior close to the free surface of the solution to the parabolic problem (3) is deduced from the property that is bounded, which gives . For the model with constant viscosity, this leads to and U has a (rather) parabolic profile close to the free surface. For the model with rheology, Equation (41) implies that I tends to a finite value as , and thus with Equation (40), we obtain , and U has a (rather) Bagnold profile close to the free surface. We conclude that in any case, the Neumann condition is recovered at the free surface, even if not enforced explicitly. For the model with the rheology, tends to zero more slowly than for the model with constant viscosity, leading to a behavior closer to the prediction of the inviscid model. Nevertheless, the property at the free surface, which seems to be a consequence of the incompressible viscoplastic model, makes it impossible to obtain a good representation of the experimental stopping phase.
Note that the
rheology was introduced precisely to represent the Bagnold profile (without a static phase)
, where
c is determined by the relation
, which gives
This Bagnold profile without a static phase is a steady solution to the system (3) and (41) with (42) and (40), but only when . In our framework, we have a static phase, the flow is not steady, and . The formula (46) is therefore not applicable and would give a negative c. Our choice of is nevertheless of the same order of magnitude as formula (46).
5. Discussion and Conclusions
We have considered the 1D (in the direction normal to the flow) non-averaged model with static/flowing dynamics that was initially proposed in [
41]. This model is based on the description of a granular material by a yield stress viscoplastic rheology. Here we have assumed that the source term in this model is constant, which corresponds to simple shear solutions to the viscoplastic model. Thus, all the quantities are assumed to be independent of the down-slope variable and in particular the flow thickness is constant. We have shown that this free interface model can be solved with reliable and relatively simple numerical methods. We have compared model solutions for both the inviscid and viscous models to observations from experiments on granular flow over an inclined static layer of grains. The analytical solution for the inviscid model and the numerical results for the viscous model reproduce quantitatively some essential features of the change with time of the velocity, of the static/flowing interface position, and of the stopping time of the granular mass, even though the flow thickness in the experiments is not perfectly uniform and the initial velocity profile changes with slope angle and flow thickness as discussed below.
The analytical solution for the inviscid model shows that the evolution of the static/flowing interface position is proportional to the source term and inversely proportional to the shear rate (Equation (9)). For the viscous model (with constant viscosity), the analysis shows that the evolution of the interface is related to the viscosity, the source term, and the first- and third-order derivative of the source term and the velocity, respectively (Equation (8)). Owing to the appearance of this third-order derivative, the dynamics of the static/flowing interface cannot be reduced to a simple differential equation in terms of depth-averaged quantities. While the shape of the initial velocity profile is preserved at all times for the inviscid model according to Equation (15), the viscous model predicts that an exponential-like tail near the static/flowing transition and a convex shape near the free surface develop. The viscous contribution enables the static/flowing interface to initially penetrate within the static layer (which is eroded), as observed in the experiments, and contrary to the inviscid model.
The viscoplastic model used here has the great advantage of involving only two parameters, i.e., the friction coefficient
and the viscosity
(or the coefficient
for the
rheology), whereas the so-called partial fluidization theory, involving an order parameter to describe the transition between static and flowing material, also reproduces the erosion of the static bed and the velocity profiles predicted here with the viscous model [
7], but at the cost of additional empirical equations for the time-change of a state parameter.
One of the important results of the analysis lies in the explicit expressions obtained from the analytical solution, especially for the time evolution of the static/flowing interface. The dynamics are controlled by the source term
S that is constant when the pressure is assumed to be hydrostatic and when the slope and thickness are assumed to be constant. In such a case,
, with
. Comparable results have been obtained from the analytical solution of thin-layer depth-averaged equations for a granular dam-break (i.e., with non-constant
h) [
43,
44]. This analytical solution predicts a granular mass front velocity that decreases linearly with time
where
(see [
9]). Furthermore, the stopping time of the analytical front for the granular dam-break is
Equations (47) and (48) for the front velocity and the stopping time of the front for a depth-averaged model of a granular dam-break are very similar to Equations (15) and (17) respectively, found here for the velocity of the flow and for the stopping time of the granular layer in the non-averaged case and without viscosity.
Although the initial penetration of the static/flowing interface into the static layer (erosion) can be reproduced by taking into account the viscosity, this leads at the same time to an underestimation of the stopping time. The viscous model better reproduces the exponential-like tail of the velocity profile near the static/flowing interface than the inviscid model, but overestimates the convexity of the velocity profile near the free surface. Furthermore, the change in shape of the velocity profile observed in the experiments during the stopping phase is reproduced by the viscous model, as opposed to the inviscid model. However, the decrease in maximum velocity near the surface is too fast in the viscous model. All these results suggest that (i) viscosity plays an important role near the static/flowing interface at depth and in this region a reasonable estimate for the viscosity is
m
s
and (ii) viscous effects in the experiments seem to be much smaller near the free surface. These observations suggest a non-constant viscosity, as proposed in the so-called
flow law, e.g., [
25,
26,
27,
28]. As in [
32], we have used the
flow law to derive the value of the viscosity, which becomes variable and nonlinear with respect to the shear rate. This flow law reproduces approximately the value of the viscosity at the static/flowing interface (i.e.,
m
s
) and at the free surface (vanishing viscosity). However, this model does not allow us to significantly improve the accuracy of the behavior of the static/flowing interface close to stopping. This is because it imposes a Bagnold behavior close to the free surface, which is in contradiction with experiments that predict a linear behavior. A more detailed numerical simulation of the granular collapse over sloping beds with the complete viscoplastic model and the
rheology gives a dynamic viscosity of around 0.2Pa· s near the front, increasing up to about 0.4Pa·s behind the front (see Figure 11 of [
33] and Figure 10 of [
32]), leading to a kinematic viscosity of
m
s
and
m
s
, respectively, for a density of
kg/m
. Note also that our treatment of side wall effects deserves further improvements, since we simply increased the friction coefficient as done in [
27,
32,
42]. Taking into account wall effects changes the static/flowing position, as shown in particular in [
33] for the granular collapse considered here. More precisely, the static/flowing interface is found to be less deep within the flow when wall effects are accounted for (see Figures 3 and 4 of [
33]). This effect could possibly increase the value of the viscosity needed in the model to reproduce the penetration of the static/flowing interface observed in the experiments. This would give values of the viscosity closer to that given by the
rheology near the front (Figure 11 of [
33]).
It would be of interest to take into account the
X-variations of the source
S from ([
41], Equation (2.12)), thereby accounting for topography, propagation and non-hydrostatic effects. This would make it possible to study erosion in flows over complex topography in the laboratory (e.g., [
45]) or at the natural scale (e.g., [
46]). For the very simple case of flows over a constant slope and if the pressure is assumed to be hydrostatic (
), taking into account the
X-variations is the same as (according to [
41]) considering once again (3)–(6) with
S including an additional term,
and as considering a thickness
that evolves according to (2.2) in [
41]. Then
and
. However
in (49) is still independent of
Z. Then Equations (8) and (9) read as follows with
defined by (49):
If
and
, then
If
and
, then
The model with
is valid as long as
, so as to satisfy (6). Indeed, violating this condition leads to instantaneous flow of the whole layer i.e.,
, and full erosion of the bed. In this case, (3) still has to be solved (with
and
), but with boundary conditions (4a) and (4c) only. If at some later time
S becomes positive again,
b can rise above the value
. Thus when
can change sign, there is in general a succession of progressive depositions and sudden full erosions of the bed. As discussed previously, the experimental granular flow is not perfectly uniform, as illustrated for example for the granular collapse at
in
Figure 17. In this case,
, so that near the front, where the
h-gradient is strongest (
s
cm
as shown in
Figure 17),
S is negative and thus even the inviscid model predicts that erosion occurs. Later, when the front flows beyond the position
cm,
decreases with values around
. Therefore
S becomes positive, and with the inviscid model, the static/flowing interface rises (i.e., deposition occurs). For the viscous model, for the case
studied in this paper, occurrence of erosion (
) or deposition (
) is related according to (50) to the change of sign of
, i.e., positive and negative, respectively. Therefore, when the
X variations are considered and under the hydrostatic assumption, the occurrence of erosion or deposition depends on the signs of both
S and
.
The influence of a
Z-dependency of
S on the static/flowing interface dynamics and on the erosion process in the free interface model (3)–(6) is studied in [
41]. It would be interesting to extend the approach proposed here to 2D and possibly 3D, so as to capture the static/flowing interface in thin-layer models, as proposed in [
40]. The orders of magnitude assumed in [
40] are indeed satisfied in the experiments discussed here, because the typical length is
m, the typical time is
s, (so that
),
m, and
m
s
, leading to
,
, and the normalized viscosity
is of the order of
or
. The primary models of [
40] with dependency on
X and without hydrostatic assumption (giving
S depending also on
Z) lead however to severe nonlinearities and ill-posedness, so that the numerical treatment of these extensions with all flow-aligned variations represents a major challenge.
An important issue is also to summarize the dynamics of the normal velocity profile using a finite number of parameters (for example the interface position b, the thickness h, and the shear rate), in order to keep computational costs low enough to simulate natural situations. This could lead to a depth-averaged model, which has until now seemed inaccessible because of the dependency on the third normal derivative in the differential Equation (8).