The conservative interaction potential
V
ss
given by Eq.
2 determines the equilibrium structural properties of the system. However, it ignores the
dynamical effect of entanglements between the arms of the star polymers, which occur predominantly at the scale of the outer blobs (further entanglements are increasingly more difficult) (Daoud and Cotton
1982; Grest et al.
1987; Likos
2006). Imagine, for example, two neighbouring star polymers which are well entangled with each other. If the distance
r
ij
between these star polymers is suddenly increased (e.g. induced by flow), the arms require some time to disentangle. This effect will become increasingly important for star polymers with increasingly long arms. During this time, there will be a transient attractive force between the star polymers. This force originates from the entanglement junctions, and it decays to zero as the arms get disentangled. Therefore, it is envisaged that the transient part Φ
t
of the interaction originates from deviations in the actual number of entanglements
n
ij
between two star polymers with respect to the equilibrium number of entanglements
n
0(
r
ij
) prevailing at the distance
r
ij
. Because, to a first approximation, the number of entanglements is expected to scale with the number of binary contacts between monomers of different star polymers, the equilibrium number of entanglements is assumed to be proportional to the overlap integral between the monomer densities of two star polymers. Placing one star at the origin and the other a distance
r
ij
displaced in the
z direction, the overlap can be calculated as:
$$ n_0(r_{ij}) \propto \int {\mathrm{d}} {\mathbf{r}} \ c({\mathbf{r}}) c({\mathbf{r}}-r_{ij} {\hat{\mathbf{e}}}_z). \label{eq_n0fromoverlap} $$
(4)
The result of a numerical calculation of the overlap integral for
f = 128 is shown in Fig.
2 (squares). The radial distribution function in Fig.
1 (circles) shows that typical pair distances are of the order of 1.5
σ (the first peak) or larger. This suggests that the nearly Gaussian part of
c(
r) for
r >
σ/2 will dominate the overlap integral for all relevant distances. Indeed, in the range
r
ij
>
σ, a reasonable fit can be made with a Gaussian dependence (dashed line in Fig.
2):
$$ n_0(r_{ij}) = n_0^{\rm amp} \exp\left( -\frac{r_{ij}^2}{\sigma^2} \right).\label{eq_n0} $$
(5)
This expression is used in the simulations, with a cutoff at
r
c
= 3
σ. The prefactor
\(n_0^{\rm amp}\) may be used to set the absolute number of entanglements. However, because only the product of
\(n_0^2\) with another parameter (
α, as explained in the next paragraph) is relevant, one of the two parameters may be set to an arbitrary value while the other is used to tune the system. Here,
\(n_0^{\rm amp}\) is set equal to 10 so that
n
0(
r
ij
) ≈ 1 at the typical distance
r
ij
= 1.5
σ of the closest neighbouring particles. In this way,
n
0(
r
ij
) can be interpreted loosely as the
fraction of the maximum number of entanglements between a pair of star polymers.
The equilibrium structure determined by
V
ss
is not perturbed if the transient part of the interactions is chosen according to van den Noort et al. (
2007):
$$ \Phi_t = \frac12 \alpha \left( n_{ij} - n_0\left( r_{ij} \right) \right)^2. \label{eq_Phit} $$
(6)
As alluded to before, we observe that only the product
\(\alpha n_0^2(r)\) is of relevance to the interaction Φ
t
. The parameter
α determines the allowed fluctuations of
n
ij
around
n
0(
r
ij
): according to the equipartition theorem, each quadratic contribution to the energy will have an average value of
\(\frac12 k_BT\); hence,
\(\big\langle \big( n_{ij} - n_0(r_{ij}) \big)^2 \big\rangle = k_BT/\alpha\). In the simulation,
α is set to 4
k
B
T. Similar to the case of the conservative interactions, the transient interactions are taken to be zero beyond the cut-off distance
r
c
= 3
σ.
A surplus or deficiency in the fraction of entanglements
\(n_{ij} \ne n_0(r_{ij})\) relaxes in the simulation as
$${\mathrm{d}} n_{ij} = - \frac{(n_{ij} - n_0(r_{ij}))}{\tau} {\mathrm{d}} t + \theta \sqrt{ \frac{2k_BT {\mathrm{d}} t}{\alpha \tau} } \label{eq_dn} $$
(7)
where the first term represents the tendency of the entanglement fraction to grow or diminish towards the equilibrium value with a characteristic time
τ, and the second term gives the noise on the transient forces (
θ is a number from a univariant normal distribution) (van den Noort et al.
2007). The characteristic time must be relatively large because the long chains in the corona take a long time to entangle or disentangle. In start-up shear experiments at
c = 1.5
c
*, overshoot is observed for shear rates ≥ 0.005 s
− 1 (Beris et al.
2008). Preliminary simulations at
c = 1.5
c
* showed that overshoots at such low shear rates arise only when the relaxation time is set sufficiently large: for
τ ≫ 1 s, all observations and conclusions remain essentially unchanged. In the simulations,
τ is set to 100 s.
The friction
ξ
i
on a particle
i for motion relative to the average flow field consists of two contributions:
$$ \xi_i = \xi_0 + \xi_e \sum\limits_j \sqrt{n_{ij} n_0(r_{ij})} \label{eq_friction} $$
(8)
where
ξ
0 is the dilute limit friction with the solvent and
ξ
e
an additional friction associated with the entanglements with other star polymers. This form ensures that there is no entanglement friction between particles beyond the cut-off
r
c
. The value of
ξ
0 is set equal to 6
πη
s
R
h
, where
η
s
≈ 0.014 Pa s is the solvent viscosity and
R
h
≈ 55 nm is the experimentally determined hydrodynamic radius. The value of
ξ
e
is set to 10
− 8 kg/s. Together with the chosen value of
α, this predicts a zero-shear viscosity and star self-diffusion coefficient at overlap concentration in agreement with experiment.