certain time $t_{c}$ (Fig. \[fig:17\]). The straight lines represent fits whose slopes match the [LLE]{} (Table \[tab:5\]). They are in inverse proportion with the onset times of chaoticity $(\tau = 1/\lambda_{Max})$, being a measure of the trajectory decoupling at a microscopic level.

[cccc]{} Oscillation frequency & $L=0$ & $L=1$ & $L=2$\
$\Omega \:_{ad} = 0.020\: c/\rm{fm}$ & $0.003939$ & $0.008689$ & $0.004306$\
$\Omega \:_{ad} = 0.050\: c/\rm{fm}$ & $0.004432$ & $0.009829$ & $0.023203$\
$\Omega \:\;\ \   = 0.100\: c/\rm{fm}$ & $0.000761$ & $0.015454$ & $0.014402$\
$\Omega _{res} = 0.145\: c/\rm{fm}$ & $0.008739$ & $0.016662$ & $0.010086$\

When the single-particle and collective *d.o.f.* remain uncoupled, the Lyapunov exponents basically oscillate between two quasi-stationary regimes. This happens for all vibrational frequencies involved, reflecting a periodical regrouping of orbits in two basins of attraction. The phase space not being covered, even after a hundred of thousand of $\rm{fm}/c$, computing the [LLE]{} becomes futile for this case.

One can remark for dipole oscillations (Fig. \[fig:17\] - middle column) a faster evolution towards reaching saturation states of the 4-dimensional Lypaunov exponents, once passing from the adiabatic $(\tau _{ad}=115\ \rm{fm}/c)$ to the resonance phase of the interaction $(\tau _{res}=60\ \rm{fm}/c)$.

In the monopolar case the intermittency 